2.1. Governing equations and input–output form

We consider a temperature stratified turbulent channel flow with periodic streamwise (${x}^{\star }$) and spanwise (${z}^{\star }$) directions, and walls located at ${y}^{\star } = \{ 0, 2{h}^{\star } \}$ (see figure 1). The net mass flux in the streamwise direction is constant, and the no-slip walls (${u}^{\star } = {v}^{\star } = {w}^{\star } = 0$) are maintained at constant but different temperatures. The top wall is $\Delta {T}^{\star }$ hotter than the bottom one, which induces a stable stratification in the vertical direction, aligned with the mean shear.

The temperature-induced density fluctuations are assumed to be small relative to the background density, and therefore, the Boussinesq approximation can be invoked. The governing equations are the incompressible NSE combined with a transport equation for the temperature field, which in non-dimensional form are

(2.1a)\begin{gather} \boldsymbol{\nabla} \boldsymbol{\cdot} \boldsymbol{u} = 0, \end{gather}

(2.1b)\begin{gather}\partial_{t} \boldsymbol{u} + \boldsymbol{u} \boldsymbol{\cdot} \boldsymbol{\nabla} \boldsymbol{u} ={-} \boldsymbol{\nabla} \tilde{p} + \frac{1}{{Re}_{b}} \nabla^2 \boldsymbol{u} + {Ri}_{b} \, T \boldsymbol{e}_y, \end{gather}

(2.1c)\begin{gather}\partial_{t} T + \boldsymbol{u} \boldsymbol{\cdot} \boldsymbol{\nabla} T = \frac{1}{{Pr} \, {Re}_{b}} \nabla^2 T . \end{gather}

These equations will collectively be referred to as ‘NSE’ hereafter. In the above expression, $\boldsymbol {u} = (u, v, w)^{\top }$ is the velocity vector, $T$ represents temperature, $t$ denotes time, $\tilde {p} = p - p_{h}$ is the difference between the kinematic pressure ($p$) and the hydrostatic pressure of the constant background density ($p_{h}$), and $\boldsymbol {e}_y$ is the unit vector in the wall-normal direction. All flow quantities are made dimensionless with the channel half-height (${h}^{\star }$), bulk velocity (${U}^{\star }_b$) and half the temperature difference between the walls ($\Delta {T}^{\star } / 2$). The resulting non-dimensional problem parameters are the Prandtl number $Pr = {\nu }^{\star } / {\kappa }^{\star }$ (where ${\nu }^{\star }$ is the kinematic viscosity and ${\kappa }^{\star }$ the thermal diffusivity of the fluid), Reynolds number ${Re}$ and Richardson number ${Ri}$. The Reynolds and Richardson numbers can be defined with respect to the bulk (${U}^{\star }_b$) or friction (${u}^{\star }_{\tau }$) velocities,

(2.2a)\begin{gather} {Re}_{b} = \frac{{U}^{{\star}}_b {h}^{{\star}}}{{\nu}^{{\star}}} ,\quad {Ri}_{b} = \frac{{\alpha}^{{\star}} \Delta {T}^{{\star}} {g}^{{\star}} {h}^{{\star}}}{2 {{U}^{{\star}}_b}^2}, \end{gather}

(2.2b)\begin{gather}{Re}_{\tau} = \frac{{u}^{{\star}}_{\tau} {h}^{{\star}}}{{\nu}^{{\star}}} ,\quad {Ri}_{\tau} = \frac{{\alpha}^{{\star}} \Delta {T}^{{\star}} {g}^{{\star}} {h}^{{\star}}}{{{u}^{{\star}}_{\tau}}^2}, \end{gather}

where ${g}^{\star }$ denotes the gravitational acceleration and ${\alpha }^{\star }$ is the thermal expansion coefficient. The majority of the results will be presented using inner scaling, and where helpful bulk quantities will be reported.

In order to classify dynamical contributions as linear or nonlinear, we rewrite (2.1) in input–output form, which leads to the so-called resolvent formulation of the NSE. Formally, any flow variable $\zeta$ is Reynolds decomposed into a spatio-temporal mean $\overline {\zeta }(y)$ and fluctuations ${\zeta }^{\prime }(x, y, z, t)$. With knowledge of the mean-flow profiles, we turn to the fluctuation equations where we group all linear terms on the left-hand side, while the nonlinear terms are isolated on the right-hand side. The fluctuation equations are Fourier transformed in the homogeneous spatial directions ($x$ and $z$) and in time, using

(2.3)\begin{equation} \hat{\zeta}_{\boldsymbol{k}}(y) = {\mathcal{F} \{ \zeta \}} = \frac{1}{2 {\rm \pi} L_{x} L_{z}} \int_{-\infty}^{\infty} \int_0^{L_x} \int_0^{L_z} \zeta(x, y, z, t) \,{\rm e}^{-{\rm i}( k_x x + k_z z - \omega t )} \, \mathrm{d} z \, \mathrm{d}\kern0.06em x \, \mathrm{d} t. \end{equation}

Due to the finite size of the domain in $x$ (with period $L_x$) and $z$ (period $L_z$), the associated wavenumbers $k_x = k (2{\rm \pi} / L_x)$ and $k_z = l (2{\rm \pi} / L_z)$ are constrained to integer multiples ($\{ k, l \} \in \mathbb {Z}$) of the fundamentals. The wavenumbers are collected in the vector $\boldsymbol {k} = (k_x, k_z, \omega )^{\top }$ and a single Fourier mode will be referred to as $\hat {\zeta }_{\boldsymbol {k}}$, where the superscript hat indicates a complex-valued quantity. Note that the sign convention in the Fourier transform of the spatial and temporal directions is different, so that a Fourier mode with positive $k_x$ and $\omega$ advects downstream at wave speed $c = \omega / k_x$.

With these manipulations, the fluctuation equations at each $\boldsymbol {k} \neq \boldsymbol {0}$ can be expressed as

(2.4)\begin{equation} - ( {\rm i} \omega \boldsymbol{\mathsf{M}} + \boldsymbol{\mathsf{L}} ) \boldsymbol{\mathsf{D}} \hat{\boldsymbol{q}}_{\boldsymbol{k}} = \boldsymbol{\mathsf{B}} \hat{\tilde{\boldsymbol{f}}}_{\boldsymbol{k}}, \end{equation}

where the state vector $\hat {\boldsymbol {q}}_{\boldsymbol {k}}$ and the nonlinear-forcing vector $\hat {\tilde {\boldsymbol {f}}}_{\boldsymbol {k}}$ are given by

(2.5a,b)\begin{equation} \hat{\boldsymbol{q}}_{\boldsymbol{k}} = \begin{pmatrix} \hat{u}_{\boldsymbol{k}} \\ \hat{v}_{\boldsymbol{k}} \\ \hat{w}_{\boldsymbol{k}} \\ \hat{T}_{\boldsymbol{k}} \end{pmatrix}, \quad \hat{\tilde{\boldsymbol{f}}}_{\boldsymbol{k}} = \begin{pmatrix} \widehat{\tilde{f}_{u}}_{\boldsymbol{k}} \\ \widehat{\tilde{f}_{v}}_{\boldsymbol{k}} \\ \widehat{\tilde{f}_{w}}_{\boldsymbol{k}} \\ \widehat{\tilde{f}_{T}}_{\boldsymbol{k}} \end{pmatrix}= \begin{pmatrix} -(\widehat{{\boldsymbol{u}}^{\prime} \boldsymbol{\cdot} \boldsymbol{\nabla} {u}^{\prime}})_{\boldsymbol{k}} \\ -(\widehat{{\boldsymbol{u}}^{\prime} \boldsymbol{\cdot} \boldsymbol{\nabla} {v}^{\prime}})_{\boldsymbol{k}} \\ -(\widehat{{\boldsymbol{u}}^{\prime} \boldsymbol{\cdot} \boldsymbol{\nabla} {w}^{\prime}})_{\boldsymbol{k}} \\ -(\widehat{{\boldsymbol{u}}^{\prime} \boldsymbol{\cdot} \boldsymbol{\nabla} {T}^{\prime}})_{\boldsymbol{k}} \end{pmatrix} = \widehat{\boldsymbol{f}_i}_{\boldsymbol{k}} + \hat{\boldsymbol{f}}_{\boldsymbol{k}}, \end{equation}

and the operators $\boldsymbol{\mathsf{M}}$, $\boldsymbol{\mathsf{L}}$, $\boldsymbol{\mathsf{D}}$ and $\boldsymbol{\mathsf{B}}$ are defined in Appendix A. The operators themselves depend on the wavenumber vector, but the subscript $\boldsymbol {k}$ is omitted for compactness. The nonlinear forcing can further be split into irrotational ($\boldsymbol {f}_i)$ and solenoidal ($\boldsymbol {f}$) parts. The former lies in the null space of the operator $\boldsymbol{\mathsf{B}}$, so that the solenoidal part alone determines the velocity response (see e.g. Chorin & Marsden Reference Chorin and Marsden1993). We will therefore replace $\hat {\tilde {\boldsymbol {f}}}_{\boldsymbol {k}}$ in (2.4) by $\hat {\boldsymbol {f}}_{\!\boldsymbol {k}}$ and only report the dynamically relevant solenoidal part of the forcing. Note that the temperature forcing is not subject to the solenoidal constraint, and therefore, $\widehat {\tilde {f}_T}_{\boldsymbol {k}} = \widehat {f_T}_{\boldsymbol {k}}$.

The operator on the left-hand side of (2.4) can be inverted to obtain the NSE in input–output form. The linear operator that maps the nonlinear forcing $\hat {\boldsymbol {f}}_{\!\boldsymbol {k}}$ (considered the input) to the flow response $\hat {\boldsymbol {q}}_{\boldsymbol {k}}$ (output) is called the resolvent operator $\boldsymbol{\mathsf{R}}$,

(2.6)\begin{equation} \hat{\boldsymbol{q}}_{\boldsymbol{k}} ={-} \boldsymbol{\mathsf{C}} ({\rm i} \omega \boldsymbol{\mathsf{I}} + \boldsymbol{\mathsf{L}}_1 )^{{-}1} \boldsymbol{\mathsf{B}}_1 \,\hat{\boldsymbol{f}}_{\boldsymbol{k}} = \boldsymbol{\mathsf{R}} \hat{\boldsymbol{f}}_{\boldsymbol{k}}, \end{equation}

where $\boldsymbol{\mathsf{L}}_1 = \boldsymbol{\mathsf{M}}^{-1} \boldsymbol{\mathsf{L}}$ and $\boldsymbol{\mathsf{B}}_{1} = \boldsymbol{\mathsf{M}}^{-1} \boldsymbol{\mathsf{B}}$; the definition of the operator $\boldsymbol{\mathsf{C}}$ is given in Appendix A. It is important to point out that the resolvent depends on the choice of input and output variables. Other definitions would be possible, for example, if the NSE were formulated in velocity–vorticity form. It should also be noted that (2.6) is an exact representation of the NSE at each $\boldsymbol {k}$ when the mean-velocity and mean-temperature profiles are known.

The resolvent formulation provides a natural partitioning of the flow dynamics and stratification effects into linear and nonlinear interpretations, as illustrated by the block diagram of figure 2. Past studies typically analyse one of the two blocks (see e.g. Morra et al. Reference Morra, Nogueira, Cavalieri and Henningson2021; Huang et al. Reference Huang, Toedtli, Chini and McKeon2023), and following this approach we focus on the lower half of the diagram. Starting from the flow response $\boldsymbol {q}_{\boldsymbol {k}}$, the present study investigates how the resolvent $\boldsymbol{\mathsf{R}}$ and nonlinear forcing $\boldsymbol {f}_{\boldsymbol {k}}$ localize internal gravity waves in spectral space and in the channel core. We will term flow features associated with the resolvent operator $\boldsymbol{\mathsf{R}}$ as linear effects, which will be studied in § 4. Phenomena associated with the forcing $\hat {\boldsymbol {f}}_{\!\boldsymbol {k}}$ will be classified as nonlinear effects, and are the subject of § 5.

Figure 2.

(a) Block diagram of the NSE in resolvent form. (b,c) Components of the CSD tensor for the flow response ($\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}}$) and forcing ($\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k}}$). (d,e) Physical flow structure of the leading forcing SPOD mode ($\hat {\boldsymbol {\chi }}_1$) and associated flow response ($\boldsymbol{\mathsf{R}} \hat {\boldsymbol {\chi }}_1$).

2.2. Data acquisition and processing

The input–output framework is applied to high-fidelity data obtained from DNS of a turbulent channel flow at ${Re}_{\tau } \approx 180$. Three conditions are considered: an unstratified case (${Ri}_{\tau } = 0$, labelled ‘R0’), which serves as a reference, and two stratified ones. The weakly stratified simulation at ${Ri}_{\tau } \approx 60$ (labelled ‘R60’) will be the main focus of this study, and the last computation at ${Ri}_{\tau } \approx 120$ (labelled ‘R120’) is analysed to verify that the results generalize to more strongly stratified flows. For a given ${Re}_{\tau }$, the feasible range of Richardson numbers is limited by the requirement that the majority of the flow stay fully turbulent, so that the Reynolds decomposition remains physically meaningful. The simulations discussed herein cover the feasible ${Ri}$ range at ${Re}_{\tau } \approx 180$, in accordance with earlier results by García-Villalba & del Álamo (Reference García-Villalba and del Álamo2011). The relevant flow parameters of all cases are summarized in table 1. The Nusselt number is defined as $Nu = {d}_{y} \overline {{T}^{\star }}|_{{y}^{\star } = 0} (2 {h}^{\star } / \Delta {T}^{\star })$ and the expressions for the other non-dimensional groups can be found in (2.2).

Table 1.

Flow parameters for unstratified (R0) and stratified flows (R60, R120).

2.2.1. Direct numerical simulation

The DNS uses a fractional step method with local volume fluxes in a staggered grid arrangement, as described in Rosenfeld, Kwak & Vinokur (Reference Rosenfeld, Kwak and Vinokur1991). The time-stepping algorithm is Adams–Bashforth for the nonlinear advection terms and Crank–Nicolson for the diffusive terms. The pressure Poisson equation is solved with Fourier transforms in the periodic streamwise and spanwise directions, leading to a tridiagonal system that can be solved efficiently. The code has been extensively validated in unstratified transitional (Marxen & Zaki Reference Marxen and Zaki2019; Wang, Wang & Zaki Reference Wang, Wang and Zaki2019a) and fully turbulent channel flows (Wang, Hasegawa & Zaki Reference Wang, Hasegawa and Zaki2019b; Wang & Zaki Reference Wang and Zaki2021), and further validation for the stratified case is presented in §§ 3 and 5.

The channel flow is driven by a constant mass flux and the bulk Reynolds number is increased with stratification, so that ${Re}_{\tau } \approx 180$ in all cases. The domain size and grid resolution are summarized in table 2. The superscript plus indicates normalization with respect to the viscous scales (${u}^{\star }_{\tau }$ and ${\nu }^{\star } / {u}^{\star }_{\tau }$), which are approximately constant across flow configurations. The grid is uniform in the streamwise and spanwise directions, and the non-uniform grid spacing in $y$ follows a stretched hyperbolic tangent function. A larger domain size is required to sustain turbulence in configuration R120, and the $\{x, z\}$ grid resolutions are reduced to keep the storage requirements feasible. The grid is only slightly coarser compared to previous DNS studies (e.g. García-Villalba & del Álamo Reference García-Villalba and del Álamo2011; Ahmed et al. Reference Ahmed, Bae, Thompson and McKeon2021); even so our analysis will put less emphasis on this coarser simulation. The time step is fixed ({R0, R60}: $\Delta t^+ = 0.045$, R120: $\Delta t^+ = 0.034$) and the total integration times are ${t}^{\star } ({u}^{\star }_{\tau } / {h}^{\star }) = \{ 210, 204, 187 \}$ for {R0, R60, R120}, respectively. A total of $10\,001$ flow snaspshots $\boldsymbol {q}(x, y, z, t)$ are collected for each configuration at a constant sampling interval of $\Delta t_s^{+} \approx \{ 3.7, 3.6, 3.4\}$, resulting in $16$ TB of data per flow condition.

Table 2.

Domain size and grid parameters. The variables $N_x$, $N_y$ and $N_z$ denote the number of grid points in each direction. Note that the horizontal domain size and grid resolution are different for case R120.

2.2.2. Data processing

The input–output relation in (2.6) is defined in Fourier space, while the DNS data are available in physical space on a staggered grid and at constant time intervals. To unify the two perspectives, a spectral representation of the DNS data is obtained in post-processing.

In a first step, the instantaneous DNS fields $\boldsymbol {q}(x,y,z,t)$ are Fourier transformed in $x$ and $z$, and spectrally upsampled to $(3/2) N_x$ and $(3/2) N_z$ wavenumbers. A complex phase shift is then applied to collocate all flow variables on the $x$ and $z$ vertices of the original spatial grid. The DNS data are subsequently interpolated from the stretched hyperbolic tangent grid in $y$ onto Chebyshev collocation points using cubic splines, with an additional zero slope constraint for $v$ at $y = \{ 0, 2\}$ to enforce continuity at the wall. The appropriate number of Chebyshev collocation points $N_c = 161$ is determined as the minimum $N$ at which the reconstruction error no longer decreases with an increasing number of collocation points. The collocated velocity fields are divergence free with respect to the finite volume numerics of the DNS, but not necessarily with respect to the spectral operators. We therefore apply a spectral Leray projector $\mathbb {P}$ to enforce incompressibility with respect to the Fourier and Chebyshev operators

(2.7)\begin{equation} \mathbb{P}(\hat{\boldsymbol{u}}_{\boldsymbol{\xi}} (y, t)) = \hat{\boldsymbol{u}}_{\boldsymbol{\xi}}(y, t) - \boldsymbol{\nabla} \Delta^{{-}1} (\boldsymbol{\nabla} \boldsymbol{\cdot} \hat{\boldsymbol{u}}_{\boldsymbol{\xi}}(y, t)), \end{equation}

where $\boldsymbol {\xi } = (k_x, k_z)^{\top }$ is the spatial wavenumber vector and $\hat {\boldsymbol {u}}_{\boldsymbol {\xi }}$ denotes the $\{ x,z \}$ Fourier coefficients of the velocity field. We have further validated that the original and projected velocity fields have the same flow statistics.

The nonlinear terms $\tilde {\boldsymbol {f}}(x, y, z, t)$, which represent the input in (2.6), are evaluated pseudo-spectrally from the divergence-free part of the collocated flow snapshots. The quadratic advection terms are evaluated in physical space and the $(3/2)$ rule is used to dealias the time-dependent spatial Fourier coefficients $\hat {\tilde {\boldsymbol {f}}}_{\boldsymbol {\xi }}(y,t)$. Recall that only the divergence-free part of the velocity forcing, $\tilde {\boldsymbol {f}}_{\!\boldsymbol {u}}$, is required for the input–output formulation in (2.6), which can be extracted with a similar Leray projector as (2.7),

(2.8)\begin{equation} \widehat{\boldsymbol{f}_{\boldsymbol{u}}}_{\boldsymbol{\xi}}(y,t) = \mathbb{P}(\,\widehat{\tilde{\boldsymbol{f}}_{\boldsymbol{u}}}_{\boldsymbol{\xi}}(y, t)). \end{equation}

The final processing step is to estimate the temporal frequency content at each $\boldsymbol {k}$ of the DNS data. To obtain converged estimates, we average over multiple realizations (Welch's method; see e.g. Towne et al. Reference Towne, Schmidt and Colonius2018), which is achieved by splitting the time series into shorter segments of $300$ samples (or time window $T_{\eta }$), with 50 % overlap between adjacent blocks; we then apply a Hann window $\eta (t)$ to each segment to enforce periodicity:

(2.9)\begin{equation} \eta(t) = \frac{\tilde{\eta}(t)}{\displaystyle\left( \dfrac{1}{T_{\eta}} \int_0^{T_{\eta}} \tilde{\eta}^2(t) \, \mathrm{d}t \right)^{1/2}}, \quad \tilde{\eta}(t) = \sin^2\left( \frac{{\rm \pi} t}{T_{\eta}} \right) \text{ for } 0 \leq t \leq T_{\eta}. \end{equation}

It is important to point out that the window function introduces additional temporal dynamics, since $\eta (t)$ does not commute with the time derivative. The window dynamics have to be accounted for in (2.6) by replacing $\hat {\boldsymbol {q}}_{\boldsymbol {k}}$ and $\hat {\boldsymbol {f}}_{\!\boldsymbol {k}}$ by

(2.10a,b)\begin{equation} \hat{\boldsymbol{q}}_{\eta \boldsymbol{k}} = \begin{pmatrix} \widehat{(u \eta)}_{\boldsymbol{k}} \\ \widehat{(v \eta)}_{\boldsymbol{k}} \\ \widehat{(w \eta)}_{\boldsymbol{k}} \\ \widehat{(T \eta)}_{\boldsymbol{k}} \end{pmatrix},\quad \hat{\boldsymbol{f}}_{\eta \boldsymbol{k}} = \begin{pmatrix} \widehat{(f_u \eta)}_{\boldsymbol{k}} + \widehat{(u {d}_{t} \eta)}_{\boldsymbol{k}} \\ \widehat{(f_v \eta)}_{\boldsymbol{k}} + \widehat{(v {d}_{t} \eta)}_{\boldsymbol{k}} \\ \widehat{(f_w \eta)}_{\boldsymbol{k}} + \widehat{(w {d}_{t} \eta)}_{\boldsymbol{k}} \\ \widehat{(f_T \eta)}_{\boldsymbol{k}} + \widehat{(T {d}_{t} \eta)}_{\boldsymbol{k}} + {d}_{y} (\overline{vT}) \hat{\eta}(\omega) \delta_{k_{x}0} \, \delta_{k_{z}0} \end{pmatrix}, \end{equation}

where $\delta _{k_x 0}$ is the Kroenecker Delta in the Fourier domain. This is an inherent limitation of analysing the temporal frequency content of non-periodic signals. All reported temporal statistics of the nonlinear-forcing terms contain the additional window dynamics, since this is required to satisfy the input–output relation equation (2.6) to satisfactory accuracy (see also Morra et al. (Reference Morra, Nogueira, Cavalieri and Henningson2021) for additional details).

2.2.3. Spectral densities

Spectral densities are used to statistically characterize the turbulence and the forcing, at individual length and time scales. The CSD tensor is an appropriate statistical characterization of the Fourier coefficients, which we compute following the algorithm by Towne et al. (Reference Towne, Schmidt and Colonius2018). The CSD of the turbulence is denoted as $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}}$ and that of the forcing is denoted as $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k}}$. Both quantities are formally defined as

(2.11a)\begin{gather} \hat{\boldsymbol{\mathsf{S}}}_{\boldsymbol{k}}(y, y^{\prime}) = \mathbb{E} [ \hat{\boldsymbol{q}}_{\eta \boldsymbol{k}}(y) \hat{\boldsymbol{q}}_{\eta \boldsymbol{k}}^H (y^{\prime}) ], \end{gather}

(2.11b)\begin{gather}\hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k}}(y, y^{\prime}) = \mathbb{E} [\, \hat{\boldsymbol{f}}_{\eta \boldsymbol{k}}(y) \hat{\boldsymbol{f}}_{\eta \boldsymbol{k}}^H(y^{\prime}) ], \end{gather}

and are shown schematically on the top right of figure 2. Note that each sub-block of $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}}$ and $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k}}$ corresponds to the covariance between different components of the state and forcing vector, respectively. All CSDs are ensemble averaged over the windowed realizations of duration $T_{\eta }$ and normalized by the wavenumber ($\Delta k_i$) and frequency ($\Delta \omega$) spacing to obtain true spectral densities. Equation (2.6) implies that the resolvent relates the CSD of the forcing and the flow response,

(2.12)\begin{equation} \hat{\boldsymbol{\mathsf{S}}}_{\boldsymbol{k}} = \mathbb{E} [ \hat{\boldsymbol{q}}_{\eta \boldsymbol{k}} \hat{\boldsymbol{q}}_{\eta \boldsymbol{k}}^H ] = \boldsymbol{\mathsf{R}} \mathbb{E} [\,\hat{\boldsymbol{f}}_{\eta \boldsymbol{k}} \hat{\boldsymbol{f}}_{\eta \boldsymbol{k}}^H ] \boldsymbol{\mathsf{R}}^H = \boldsymbol{\mathsf{R}} \hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k}} \boldsymbol{\mathsf{R}}^H. \end{equation}

This input–output relation can be used to verify the convergence and accuracy of the right-hand side in comparison to direct computation of the left-hand side; (2.12) further provides a framework to analyse the flow response generated due to subsets of the forcing $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k}}$. Both aspects will be explored in § 5.

The real-valued diagonal terms of the CSD tensors are of particular interest and will be used to illustrate the flow structure at specific $\boldsymbol {k}$. The diagonal terms are referred to as power spectral densities (PSDs) and are denoted by a corresponding lower-case symbol, with the component indicated in the subscript (for example, $\boldsymbol {s}_{\boldsymbol {k} vv}$ and $\boldsymbol {p}_{\boldsymbol {k} vv}$). The integral of the PSD over $\omega$ recovers the time-averaged PSD (denoted by $\boldsymbol {s}_{\boldsymbol {\xi } vv}$, $\boldsymbol {p}_{\boldsymbol {\xi } vv}$, etc.) and the integral over $\boldsymbol {k}$ is equal to the variance.

3.1. Mean profiles

Select ensemble-averaged statistics are presented in figure 3. The solid lines correspond to the present DNS, with stronger stratification represented by darker lines, while the open symbols are data from the simulations by Ahmed et al. (Reference Ahmed, Bae, Thompson and McKeon2021). The profiles are either anti-symmetric (mean temperature $\overline {T}$) or symmetric (remaining quantities) about the channel centreline, and only the data in the lower channel half $y \in [0, 1]$ are reported. All quantities show good agreement with the data by Ahmed et al. (Reference Ahmed, Bae, Thompson and McKeon2021), which confirms the accuracy of our simulations.

Figure 3.

Spatio-temporal mean profiles for different flow configurations. Case R0 (unstratified), light blue; case R60, medium blue; and case R120, dark blue. Lines represent the current simulations, while symbols outline data of Ahmed et al. (Reference Ahmed, Bae, Thompson and McKeon2021). (a) Mean streamwise velocity, (b) mean temperature, (c) r.m.s. of wall-normal velocity, (d) r.m.s. of solenoidal wall-normal velocity forcing, (e) r.m.s. of temperature, (f) r.m.s. of temperature forcing.

The modifications of the mean and r.m.s. velocity and temperature profiles (figure 3a–c,e) due to gravity effects have been extensively discussed by García-Villalba & del Álamo (Reference García-Villalba and del Álamo2011) and we only summarize a few key observations. The near-wall turbulence is little affected by stable stratification and the profiles collapse in this region when normalized by viscous scales. The largest modifications are observed close to the channel centre, where the mean-velocity profile approaches a parabola and the mean-temperature gradient steepens with increasing ${Ri}$. The wall-normal velocity fluctuations decrease with stratification in the region $0.5 < y < 0.9$ and recover the unstratified level only close to the channel centre. In contrast, stratification increases the temperature fluctuations beyond the near-wall region. The largest fluctuations are recorded in the channel centre for R60, and reduce slightly for stronger stratification. It is important to remark that the temperature fluctuations are normalized by the friction temperature ${T}^{\star }_{\tau } = ({\kappa }^{\star } / {u}^{\star }_{\tau }) \, {d}_{y} \overline {{T}^{\star }}|_{{y}^{\star }= 0}$, which decreases with stratification (compare the Nusselt numbers in table 1) and, thus, magnifies the r.m.s. profile at higher ${Ri}$. Independent of normalization, large $v$ and $T$ fluctuations are observed in the stratified flow close to the channel centreline, and are typically attributed to the internal gravity waves that occur in this region (García-Villalba & del Álamo Reference García-Villalba and del Álamo2011).

Figure 3(d,f) shows statistics of the nonlinear terms (forcing in the terminology of the input–output framework) of the momentum and temperature equations. As noted in § 2.1, only the dynamically relevant solenoidal part of the momentum forcing is shown. The r.m.s. fluctuations of the $v$ forcing (figure 3d) increase with ${Ri}$ except very near the channel centre, in contrast with the observed decrease in $v_{rms}$. As for the r.m.s. temperature forcing (figure 3f), it appreciably exceeds the unstratified curve beyond the near-wall region, even at values of $y$ where $T_{rms}$ is inappreciably modified. It is important, however, to keep in mind that the comment regarding the normalization by ${T}^{\star }_{{\tau }}$ is relevant here as well.

The ensemble-averaged statistics illustrate that stratification acts non-uniformly across the channel. A primary reason is that the strength of gravity effects relative to shear depends on the distance from the wall, leading to flow regions with distinct dynamics and flow characteristics. The relative strength of gravity and shear can be quantified by the gradient Richardson number,

(3.1)\begin{equation} {Ri}_g = \frac{{{N}^{{\star}}}^2}{({d}_{y} {\overline{u}}^{{\star}})^2} = \frac{{g}^{{\star}} {\alpha}^{{\star}} {d}_{y} {\overline{T}}^{{\star}}}{({d}_{y} {\overline{u}}^{{\star}})^2} = \left( \frac{{T}^{{\star}}_S}{{T}^{{\star}}_B} \right)^2, \end{equation}

which is a ratio between the time scales of local shear (${T}^{\star }_{S}$) and buoyancy (${T}^{\star }_{B}$). The latter is defined in terms of the buoyancy frequency ${{N}^{\star }}^2 = {g}^{\star } {\alpha }^{\star } {d}_{y} {\overline {T}}^{\star }$. The gradient Richardson numbers in our stratified simulations are shown in figure 4. In both cases, ${Ri}_g$ is small in proximity of the wall, which means that shear dominates over buoyancy. This implies that the near-wall flow is inappreciably affected by stratification, consistent with the agreement of the mean profiles from the stratified and unstratified flows over that region in figure 3. At higher $y$, the gradient Richardson number monotonically increases and ultimately diverges since the mean shear vanishes at the channel centreline, and gravity effects become dominant in this region. For our subsequent analysis, we divide the channel into three qualitative regions, which are indicated by different shadings in figure 4: inner region (represented in grey), outer region (no shading) and core region (green shading). The extent of the inner region will be discussed subsequently, while the boundary between the outer and core region is taken at $y = 0.8$, in accordance with Lloyd et al. (Reference Lloyd, Dorrell and Caulfield2022).

Figure 4.

Gradient Richardson number of the stratified flows. The shaded areas indicate the different conceptual layers in the lower half of the channel. Grey, inner region; white, outer region; green, core region.

3.2. Time-averaged PSDs

The mean profiles of the previous section provide a global sense of flow modification by stratification. In contrast, the input–output view of the NSE (figure 2) is formulated for individual wavenumber triplets and a suitable $\boldsymbol {k}$ has to be chosen to proceed with the analysis. The choice of $\boldsymbol {k}$ is guided by the spectra of the flow response, which delineate the stratification effect at each scale, and with a focus on the channel core where stratification effects are strongest. We will emphasize the wall-normal velocity and temperature in our discussion: these variables are directly coupled by stratification (see (2.1)), admit wave-like solutions to the linearized temperature equation and most clearly show the imprint of internal gravity waves in fully turbulent flows. We first consider time-averaged PSDs, which will inform the selection of the streamwise ($k_{x}$) and spanwise wavenumber ($k_{z}$). Section 3.3 will present temporal PSDs to guide the choice of $\omega$. For conciseness, the discussion focuses on cases R0 and R60; a summary of the relevant spectra for R120 will be given in § 5.4.

Figure 5 shows the time-averaged PSD of $v$ and $T$ (figure 5a,c), as well as their forcing terms (figure 5b,d). The spectra are integrated over $k_x$ and recover the square of the fluctuations in figure 3 when integrated over the spanwise wavenumbers. Note that only a subset of the resolved $k_{z}$ is shown for clarity. Each spectrum is normalized by its maximum value (indicated above the figure) and the same contour levels $\boldsymbol {s}_{\boldsymbol {\xi }} / \max \boldsymbol {s}_{\boldsymbol {\xi }} = \{ 0.25, 0.5, 0.75 \}$ are shown for case R0 (light blue) and R60 (colour contours). We first discuss how the response and forcing PSDs change with stratification, and then contrast the spectral content of the input and output variables.

Figure 5.

Time-averaged PSDs as a function of the wall-normal coordinate $y$ and spanwise wavenumber $k_z$. The spectra are integrated over the streamwise wavenumber $k_x$ and normalized by their respective maximum value, which is reported above each figure in order {R0 (light blue), R60 (medium blue)}. The contour lines label $\boldsymbol {s}_{\boldsymbol {\xi }} / (\max \boldsymbol {s}_{\boldsymbol {\xi }}) = \{ 0.25, 0.5, 0.75 \}$ and the green vertical line denotes $k_z = 2$.

For both flows, structures with large spanwise extent (low $k_{z}$) contribute most to the variance of $v$ and $T$. In the unstratified case, the wide structures are energetic over a large part of the channel height, while stratification localizes them in the core region. This effect is most evident in the temperature (figure 5c), where stratification effectively suppresses the tall lobes that reach into the inner region of the unstratified channel.

The spanwise spectra of the forcing are more broadband in both flows (figure 5b,d), especially for $f_{v}$ where the peak in the outer flow extends across all shown wavenumbers. Interestingly, the spectral structure of $f_{v}$ is qualitatively unchanged with stratification, except perhaps in the channel core where stratification suppresses the forcing. The spectral structure of the temperature forcing, on the other hand, is significantly affected by gravity effects. The unstratified flow shows a peak that extends across the inner and outer regions, and across a broad range of $k_{z}$. Stratification significantly weakens the peak close to the wall, and instead energizes the small spanwise wavenumbers in the channel core, similar to the response spectra. This localization is much more apparent compared to the r.m.s. profile in figure 3(f), which showed a plateau in the core region.

We next compare the forcing and response spectra. It is apparent that the two are energetic in different regions. The forcing has broader support in $k_z$, which is perhaps not surprising since the nonlinear terms contain spatial gradients that amplify the small scales and triadic interactions can transfer energy across spatial scales (see e.g. Bolotnov et al. Reference Bolotnov, Lahey, Drew, Jansen and Oberai2010; Atoufi, Scott & Waite Reference Atoufi, Scott and Waite2021). From the input–output perspective of (2.4) and figure 2, it is interesting to note that the strong forcing at large $k_z$ does not translate into a significant flow response, in particular for $v$. This suggests that the linear dynamics act as a spectral filter that admits only a narrow band of wavenumbers in the response, an aspect that will be explored in more detail in § 4.3. Moreover, the wall-normal peak of the $v$ forcing occurs in the outer region, while all other displayed components peak in the channel core. This raises the question of whether forcing in both wall-normal regions is required to localize the flow response, which will be addressed in § 5.1.

To proceed with the input–output analysis, we identify a suitable $k_{x}$ and $k_{z}$ from the time-averaged spectra. Recall from § 3.1 that the gravity effects are strongest in the core region, so that the energetic scales at this $y$ are the natural choice. Moreover, we base the choice on the flow response rather than the forcing, since the former is the physically observable quantity. The most energetic spanwise wavenumber for both $v$ and $T$ is $k_{z} = 1$, which corresponds to $\lambda _z = 2 {\rm \pi}$. Since the spanwise size of the computational domain for cases {R0, R60} is $L_{z} = 2{\rm \pi} $ (see table 2), this is the fundamental wavenumber of the DNS. To preclude a possible influence of the finite domain size, it is preferable to choose a different scale and we therefore select the second most energetic scale $k_{z} = 2$, which is indicated by the green vertical line in figure 5.

The PSDs discussed in this section are integrated over $k_{x}$, and the contributions from individual streamwise wavenumbers to $k_{z} = 2$ must be considered to select a suitable $k_{x}$. For conciseness, a detailed discussion of the PSD at $k_z = 2$ is omitted, but can be found in Appendix B. We only note that the most energetic scale of the temperature response, which guides the selection, occurs at $k_x = 2$. Our subsequent analysis will therefore focus on the Fourier mode with spatial wavenumbers $\boldsymbol {\xi }_{G} = (k_x = 2, k_z = 2)^{\top }$. This wavenumber combination falls within the range typically associated with internal gravity waves (see e.g. García-Villalba & del Álamo Reference García-Villalba and del Álamo2011) and is therefore given the subscript ‘$G$.’ Our subsequent analysis will provide further evidence that $\boldsymbol {\xi }_{G}$ indeed represents the gravity waves found in the core of the stratified channel.

3.3. Temporal PSDs

This section presents the temporal PSDs of the flow response and forcing, and informs the choice of an appropriate temporal frequency $\omega$ for subsequent analysis. The discussion focuses on the temporal PSDs (diagonal entries of the CSDs), with emphasis on the wall-normal velocity and the temperature.

The PSD of $v$, $T$ and their forcing components are shown in figure 6 as a function of the wall-normal velocity and wave speed $c = \omega / k_x$. As before, the contour levels indicate $\boldsymbol {s}_{\boldsymbol {k}} / \max \boldsymbol {s}_{\boldsymbol {k}} = \{ 0.25, 0.5, 0.75 \}$ for the unstratified (light blue contour lines) and stratified (colour contours) flows, and the maximum value is indicated above each figure. In addition, the figures also show the mean-velocity profiles $\overline {u}$ of the unstratified (dashed light blue line) and stratified (dashed medium blue line) flows, for reference. The computations of the forcing PSD are the most challenging to converge and contain high-frequency noise, which is removed by a Gaussian filter to aid the interpretation.

Figure 6.

Temporal PSD of the Fourier mode $\boldsymbol {\xi }_{G}$. The PSDs in (a–d) are normalized by their maximum value, which is reported above each figure in order {R0 (light blue), R60 (medium blue)}. The contour lines label $\boldsymbol {s}_{\boldsymbol {k}} / (\max \boldsymbol {s}_{\boldsymbol {k}}) = \{ 0.25, 0.5, 0.75 \}$, the dashed lines indicate the mean-velocity profiles and the medium blue triangles denote the wave speed of the gravity waves according to the empirical relation of Lloyd et al. (Reference Lloyd, Dorrell and Caulfield2022). The green vertical line corresponds to $c^+ = 21$, which will be analysed subsequently, and the dotted horizontal line marks the associated critical-layer height ($y \approx 0.53$).

The PSD of the $v$ and $T$ response are shown in figure 6(a,c), respectively. The change in wall-normal localization with stratification is congruent with the spatial spectra at $\boldsymbol {\xi }_{G}$. Our focus here is on the localization in wave speed, which changes significantly between the two flows. In the unstratified case, the most energetic structures in the channel core advect at approximately the local mean velocity, consistent with the $k_{x}$-$\omega$ spectra of Lloyd et al. (Reference Lloyd, Dorrell and Caulfield2022). Stratification increases the mean velocity in the channel centre (compare the two dashed lines) and it is apparent that the energetic structures at ${Ri}_{\tau } = 60$ advect at a higher speed as well. However, their advection speed is significantly different from the mean velocity, which is indicative of internal gravity waves with a distinct dispersion relation. Lloyd et al. (Reference Lloyd, Dorrell and Caulfield2022) proposed an empirical dispersion relation, denoted $\tilde {c}$, for internal gravity waves in channel flow at higher Reynolds and Richardson numbers (${Re}_{\tau } \approx 550$ and ${Ri}_{\tau } = 480$), and found that

(3.2)\begin{equation} \tilde{c} = \overline{u}_{mean} \pm \frac{N_{mean}}{k_{x}} \end{equation}

provided a satisfactory fit. The subscript ‘mean’ in the above expression indicates that the mean velocity and buoyancy frequency are averaged over the channel core $y \in (0.8, 1.2)$. The two wave speeds that result from this dispersion relation are marked by the two medium blue triangles on top of each PSD. The most energetic wave speeds of $v$ and $T$ agree well with the slower of the two wave speeds from (3.2), which reinforces the evidence that $\boldsymbol {\xi }_{G} = (k_{x} = 2, k_{z} = 2)^{\top }$ is a buoyancy-driven internal gravity wave. Lloyd et al. (Reference Lloyd, Dorrell and Caulfield2022) also observed a weak gravity wave at the faster wave speed, which is not apparent in our data. This difference may be attributed to the different flow conditions of the two studies. We further note that the PSDs of the unstratified and stratified response can be approximately collapsed when plotted in frames that move at the slower of their respective wave speeds $\tilde {c}$.

Figure 6(b,d) shows the PSDs of the $v$ and $T$ forcing, respectively. The spectral energy content of the $v$ forcing changes again very little with stratification, except for a slight tilt towards higher wave speeds in the core region. The modifications of the $T$ forcing PSD are more pronounced and, similar to the spatial spectra, we observe an attenuation of the inner peak due to stratification. The stratified temperature forcing is localized in the channel core, around the same wave speed as the flow response.

For further analysis, we select the wave speed corresponding to the energetic response in the stratified channel core. This value is $c^{+} \approx 21$, which corresponds to the peak in the temperature response, and is marked by a green vertical line in figure 6. The associated critical-layer height, where $\bar {u}^{+}(y) = c^+$, is located at $y \approx 0.53$ and is marked by the horizontal dotted line in figure 6. This completes the analysis of the DNS spectra and the scale selection. In the following sections we study mode $\boldsymbol {k}_{G} = (k_{x} = 2, k_{z} = 2, c^{+} = 21)^{\top }$ for case R60 from an input–output perspective.

4.1. Linear amplification and choice of energy norm

Dominant linear amplification mechanisms at each $\boldsymbol {k}$ and their dependence on stratification can be obtained from an SVD of the resolvent operator. The SVD identifies forcing structures (inputs) that are maximally amplified by the linear dynamics (resolvent) and provides the associated flow response (output).

The notion of maximal amplification depends on the measure of the response size, which implies an appropriate choice of norm. For a physically meaningful measure, we adopt the total energy norm, which in a stratified flow is a combination of kinetic and available potential energy. The latter is defined relative to a minimum potential energy state, at which temperature (density) perturbations can no longer be converted into kinetic energy (Winters et al. Reference Winters, Lombard, Riley and Dásaro1995). In the transition literature, the laminar solution with a linear temperature profile is commonly used as a reference state (see e.g. Kaminski, Caulfield & Taylor Reference Kaminski, Caulfield and Taylor2014). In contrast, the present input–output framework defines fluctuations relative to the turbulent mean flow rather than the laminar base state. For consistency, the available potential energy has to be defined relative to the turbulent mean, so that the total fluctuation energy approaches zero as the fluctuations vanish.

With the turbulent mean as reference state, the non-dimensional expression for the energy inner product $({\cdot }, {\cdot })_E$ and associated energy norm $\lVert {\cdot } \rVert _E$ is

(4.1)\begin{equation} \lVert \hat{\boldsymbol{q}}_{\boldsymbol{k}} \rVert^2_E = (\hat{\boldsymbol{q}}_{\boldsymbol{k}}, \hat{\boldsymbol{q}}_{\boldsymbol{k}})_E = \int_{0}^2 \lvert \hat{u}_{\boldsymbol{k}} \rvert^2 + \lvert \hat{v}_{\boldsymbol{k}} \rvert^2 + \lvert \hat{w}_{\boldsymbol{k}} \rvert^2 + \frac{{Ri}_{b}}{{d}_{y} \overline{T}} \lvert \hat{T}_{\boldsymbol{k}} \rvert^2 \, \mathrm{d}\kern0.05em y \approx \hat{\boldsymbol{q}}_{\boldsymbol{k}}^H \boldsymbol{\mathsf{W}} \hat{\boldsymbol{q}}_{\boldsymbol{k}}, \end{equation}

where $\boldsymbol{\mathsf{W}}$ is the discrete weight matrix that contains the appropriate relative weights of the state variables as well as the numerical quadrature weights. The relative weight between kinetic and available potential energy is inversely proportional to the mean-temperature gradient. This dependence originates from a Lagrangian argument, which relates local perturbations in the available potential energy to vertical displacements of fluid parcels (Gill Reference Gill1982). The energy norm (4.1) is well defined so long as the mean-temperature profile is monotonically increasing or, equivalently, ${Ri}_g \geq 0$ throughout the flow. Under this condition, (4.1) provides a generalization of the energy norm used in the stratified transition literature and in previous resolvent analyses (Ahmed et al. Reference Ahmed, Bae, Thompson and McKeon2021) and recovers the latter if the laminar base flow with linear temperature profile is used. Figure 4 confirms that the temperature profiles of cases R60 and R120 are indeed monotonically increasing and that the energy norm is well defined in the present case.

For consistency with the processed DNS data, the resolvent operator is discretized on $N_c = 161$ Chebyshev collocation points and the $y$ derivatives are approximated with Chebyshev differentiation matrices (see Weideman & Reddy Reference Weideman and Reddy2000 for details on the implementation). The energy norm is enforced by weighting the resolvent operator, as described, for instance, in Luhar, Sharma & McKeon (Reference Luhar, Sharma and McKeon2014a). The SVD of the discretized and weighted resolvent returns left singular vectors $\hat {\boldsymbol {\psi }}_j$ (also termed response modes), right singular vectors $\hat {\boldsymbol {\phi }}_j$ (forcing modes) and singular values $\sigma _j$. Both sets of singular vectors are orthonormal with respect to the energy norm and form a basis for their respective spaces. The nonlinear forcing can be expanded in terms of the right singular vectors,

(4.2)\begin{equation} \hat{\boldsymbol{f}}_{\boldsymbol{k}} = \sum_j \underbrace{(\hat{\boldsymbol{\phi}}_j, \hat{\boldsymbol{f}}_{\boldsymbol{k}})_E}_{=\hat{b}_j} \, \hat{\boldsymbol{\phi}}_j, \end{equation}

with complex-valued projection coefficients $\hat {b}_j$. Similarly, the flow response and action of the resolvent operator can be written in terms of the response modes

(4.3)\begin{equation} \hat{\boldsymbol{q}}_{\boldsymbol{k}} = \boldsymbol{\mathsf{R}} \hat{\boldsymbol{f}}_{\boldsymbol{k}} = \sum_j \sigma_j \hat{b}_j \hat{\boldsymbol{\psi}}_j. \end{equation}

Equation (4.3) illustrates that the singular values represent the energy amplification of each forcing direction by the resolvent. A unit forcing aligned with the direction $\hat {\boldsymbol {\phi }}_{j}$ generates a flow response in the direction of $\hat {\boldsymbol {\psi }}_{j}$ with total energy $\sigma _j^2$. It is common practice to arrange the indices in order of descending $\sigma _j$, so that the first basis pair describes the linearly most amplified forcing and response direction.

Our subsequent analysis will investigate whether spectral regions of large $\sigma _1$ coincide with energetic regions in the full nonlinear flow, and whether the dominant left singular vectors $\hat {\boldsymbol {\psi }}_1$ give a good representation of the observed flow structures.

4.2. Localization in wavenumber space

The PSDs in § 3 revealed that the forcing and flow response are energetic at different wavenumbers and wave speeds. The forcing is more energetic at smaller streamwise and spanwise scales compared to the response (figure 5, and figure 21 in Appendix B). In addition, the forcing peaks at lower $c$ than the flow response, especially for the wall-normal velocity (see figure 6). Since the forcing and response CSDs are related through the resolvent operator (see (2.12)), this mismatch in energetic spectral regions may suggest that the linear dynamics act as a selective spectral filter when generating $\hat {\boldsymbol {q}}_{\boldsymbol {k}}$ from $\hat {\boldsymbol {f}}_{\!\boldsymbol {k}}$ (see the lower half of the block diagram in figure 2).

We explore this aspect for one of the spectral coordinates, the wave speed $c$, in figure 7. The figure shows the dominant energy amplification due to the resolvent (square of the largest singular value $\sigma _1$) at the spatial wavenumber combination $\boldsymbol {\xi }_{G} = (k_x = 2, k_z = 2)^{\top }$ as a function of the wave speed $c$ for cases R0 (light blue) and R60 (medium blue). The ordinate is shown in logarithmic scale and the diamonds at the top of the figure indicate the wave speed at which the maximum in the temperature PSDs occurs in figure 6. For the unstratified flow, the largest singular value reaches a maximum value around $c^+ \approx 17$ and drops several orders of magnitude for smaller and larger $c$. This narrow amplification peak may be interpreted as a spectral bandpass filter, which can localize the flow response in a compact spectral region from a possibly broadband flow forcing. This interpretation is indeed supported by the unstratified PSDs in figure 6. For example, consider the wave speed $c^+ = 10$, where the unstratified velocity and temperature forcings contain significant energy in the near-wall region. This forcing is only amplified by a factor of 100 by the linear dynamics, which is more than two orders of magnitude less than the peak amplification. Consistent with the low amplification, the flow response at $c^+ = 10$ is weak, well below 25 % of the maximum. On the other hand, the forcing at $c^+ = 17$ is maximally amplified by the linear dynamics, and the response PSDs peak around this same wave speed (see light blue diamond in figure 7), suggesting that the linear dynamics play a key role in the localization. It is important to keep in mind that these arguments are qualitative, because the PSDs shown in figure 6 are only a fraction of the input–output relation equation (2.12). But even so, the close correspondence between the peaks in the response PSD and energy amplification support that the linear dynamics localize the flow response in spectral space.

Figure 7.

Largest linear energy amplification for configurations R0 (light blue) and R60 (medium blue). The diamonds at the top of the figure indicate the wave speed at which the maxima occur in the temperature PSD of figure 6.

The same wavenumber localization mechanism is active for the stratified flow response, as can be seen by comparing the medium blue curve to the colour contours of the response and forcing PSDs in figure 6. In addition, the resolvent captures the shift in the dispersion relation due to the internal gravity waves in the stratified flow. The maximum $\sigma _1^2$ at ${Ri}_{\tau } = 60$ occurs at $c^+ \approx 21$, which is significantly lower than the centreline velocity of the stratified flow and agrees with the most energetic structures observed in the DNS (medium blue diamond in figure 7).

Finally, it is important to keep in mind that the integral of $\boldsymbol {s}_{\boldsymbol {k}}$ over $\omega$ recovers the time-averaged PSDs. Similar amplification plots can thus be made for other wavenumber combinations, and give insight into the spectral filtering across $\boldsymbol {k}$, which was already observed in figure 5 and figure 21 (Appendix B) for the homogeneous spatial directions.

4.3. Linearly most amplified mode shapes and their relation to DNS statistics

We next examine whether the linearly most amplified directions, or the left singular vectors $\hat {\boldsymbol {\psi }}_j$, can reproduce aspects of the DNS flow statistics. This question has been studied extensively in unstratified flows (e.g. Moarref et al. Reference Moarref, Jovanović, Tropp, Sharma and McKeon2014; Zare et al. Reference Zare, Jovanović and Georgiou2017; Towne et al. Reference Towne, Schmidt and Colonius2018; Morra et al. Reference Morra, Nogueira, Cavalieri and Henningson2021). Therefore, we limit the analysis to the stratified channel at ${Ri}_{\tau } = 60$, and focus on the buoyancy-dominated core region and mode $\boldsymbol {k}_{G} = (k_x = 2, k_z = 2, c^+ = 21)^{\top }$ that is representative of the internal gravity waves.

The compactness of the expansion equation (4.3) is indicative of how well the linearly amplified structures capture the true flow. This compactness is explored in figure 8. From (4.3), the expansion coefficients are the product of $\sigma _j$, which can be obtained from the resolvent, and the projection coefficients $\hat {b}_j$ whose statistics can be calculated from the nonlinearity. Since the temporal frequency content is estimated from a finite time series, the projection coefficients have to be interpreted in a stochastic sense and their statistics can be related to the discretized forcing CSD,

(4.4)\begin{equation} \mathbb{E} [ b_i b_j^{{\ast}} ] = \hat{\boldsymbol{\phi}}_i^H \boldsymbol{\mathsf{W}} \mathbb{E} [\,\hat{\boldsymbol{f}}_{\eta \boldsymbol{k}} \hat{\boldsymbol{f}}_{\eta \boldsymbol{k}}^H ] \boldsymbol{\mathsf{W}} \hat{\boldsymbol{\phi}}_j = \hat{\boldsymbol{\phi}}_i^H \boldsymbol{\mathsf{W}} \hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k}} \boldsymbol{\mathsf{W}} \hat{\boldsymbol{\phi}}_j, \end{equation}

which follows directly from the definition in (4.2). The decay of the singular values (black squares in figure 8) indicates that the linear dynamics act as a selective filter not only in wavenumber space. Only a handful of singular vectors (wall-normal basis functions) are amplified, and $\sigma _j$ drops by more than a decade for $j > 5$, consistent with the findings by Ahmed et al. (Reference Ahmed, Bae, Thompson and McKeon2021). In contrast, the nonlinear projection coefficients (blue triangles) increase with $j$ and counteract the filtering by the linear dynamics. Consequently, the expansion coefficients of $\hat {\boldsymbol {q}}_{\boldsymbol {k}}$ themselves (red circles) still decay, but more slowly than the singular values alone. Taken together, figure 8 indicates that a superposition of multiple left singular vectors with weights set by the nonlinearity is likely required to represent the structure of the internal gravity waves.

Figure 8.

Singular values $\sigma _j$, absolute value of projection coefficients $|\hat {b}_j|$, and their product for the stratified resolvent operator at $\boldsymbol {k}_{G}$.

This notion is made more precise by comparing the weighted resolvent modes to the DNS statistics. Figure 9 shows the absolute value of the wall-normal velocity and temperature components for the first two left (flow response) and right singular vectors (flow forcing). The figure also shows the true amplitude of the flow response and forcing at $\boldsymbol {k}$, observed in DNS, which corresponds to the square root of the PSDs along the green vertical line in figure 6. The first left singular vector reproduces the DNS flow response remarkably well in the channel core, but is less satisfactory in the outer and near-wall regions. In contrast, the second resolvent response mode is anti-symmetric across the centreline and has more support in the outer region. This and higher modes (see expansion coefficients in figure 8) are necessary to obtain the correct statistics. The relative weight and phase of the left singular vectors in the superposition is set by the nonlinearity and interested readers may refer to Appendix C for a quantitative assessment of this aspect.

Figure 9.

Absolute value of $\hat {v}_{\boldsymbol {k}}$, $\hat {T}_{\boldsymbol {k}}$ and their nonlinear forcing at $\boldsymbol {k}_{G}$. The solid black lines represent DNS data, while the dashed and dash-dotted lines denote the properly weighted first and second resolvent response and forcing modes.

The close resemblance between the DNS response profiles and left singular vectors should be contrasted with the poor agreement between right singular vectors and DNS forcing statistics (right column of figure 9). Many singular vectors would be required to reproduce the DNS forcing, and the resolvent does not provide an efficient basis (in the sense of compact representation) for the nonlinear terms. This is consistent with the initial increase and subsequent plateau of $\hat {b}_j$ in figure 8. The present results thus show that the majority of the nonlinear forcing in the channel core is not aligned with the leading resolvent forcing modes despite their associated left singular vectors being aligned with the flow response. An alternative approach to analysing the forcing is therefore desirable, which will be explored in § 5.

5.1. Three-layer structure

The PSDs of figure 6 show that the nonlinear forcing at wavenumber combinations associated with internal gravity waves spans the entire channel height and is strongest in the core. The relevance of the forcing in different wall-normal regions is explored in this section. Specifically, we divide the channel into a core, outer and inner region (as demarcated in figures 1 and 4) and quantify the contribution of the forcing in each region to the internal gravity waves. The core region is taken from the channel centre to $y = 0.8$, similar to Lloyd et al. (Reference Lloyd, Dorrell and Caulfield2022); the inner layer extends from the wall up to $y = 0.3$ for case R60. The height of this layer requires further justification, which will be given in this section.

Earlier studies used mechanistic arguments and linearized flow models to explain the generation of gravity waves in the channel core by disturbances that originate in the outer region (Lloyd et al. Reference Lloyd, Dorrell and Caulfield2022). In the present study we can quantify the contribution of the forcing at different $y$ exactly, by splitting the forcing CSD according to the three-layer structure and studying the associated flow response. Formally, we split $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k}}(y, y^{\prime })$ into sub-matrices based on the values of $y$ and $y^{\prime }$. For example, to isolate the effect of forcing in the core region, we split each component of the forcing CSD at $\{ y, y^{\prime } \} = 0.8$ and $1.2$. The first matrix, denoted $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k} | CC}$, contains all entries for which both $y$ and $y^{\prime }$ are located in the core region of the channel. In other words,

(5.1)\begin{equation} \hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k} | CC}(y, y^{\prime}) = \begin{cases} \hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k}}(y, y^{\prime}) & \text{if } y \in (0.8, 1.2) \text{ and } y^{\prime} \in (0.8, 1.2) ,\\ \boldsymbol{0} & \text{otherwise}. \end{cases} \end{equation}

The second sub-matrix is denoted $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k} | OO}$ and contains non-zero entries when both $y$ and $y^{\prime }$ lie in the near-wall or outer regions of the channel. For the lower channel half, this translates to $y \in [0, 0.8]$ and $y^{\prime } \in [0, 0.8]$, and an analogous range can be defined for the upper channel half. The last sub-matrix $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k} | CO}$ contains terms for which $y$ is located in the core and $y^{\prime }$ in the outer/near-wall region, or vice versa. By construction, the sum of the three sub-matrices recovers the full forcing CSD,

(5.2)\begin{equation} \hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k}} = \hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k}|CC} + \hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k}|OO} + \hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k}|CO}. \end{equation}

Since the input–output relation equation (2.12) is linear in $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k}}$, each sub-block generates an associated flow response,

(5.3)\begin{equation} \hat{\boldsymbol{\mathsf{S}}}_{\boldsymbol{k}} = \hat{\boldsymbol{\mathsf{S}}}_{\boldsymbol{k}|CC} + \hat{\boldsymbol{\mathsf{S}}}_{\boldsymbol{k}|OO} + \hat{\boldsymbol{\mathsf{S}}}_{\boldsymbol{k}|CO}, \end{equation}

where, for example, $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}|CC} = \boldsymbol{\mathsf{R}} \hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k}|CC} \boldsymbol{\mathsf{R}}^H$. In similar fashion, the forcing CSD can be split at a different $y$ and $y^{\prime }$ to isolate the effect of forcing in the inner layer.

We first isolate the forcing in the core and split the CSD at $\{ y, y^{\prime } \} = 0.8$ and $1.2$. The flow response to the different forcing sub-matrices is shown in figure 11 and following our earlier approach, the analysis focuses on the PSD of the wall-normal velocity and the temperature. The largest contribution to the flow response (solid black curve $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}}$) comes indeed from the forcing in the near-wall and outer regions (dash-dotted blue curve $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}|OO}$), consistent with the work by Lloyd et al. (Reference Lloyd, Dorrell and Caulfield2022). The strong nonlinear forcing in the channel core on the other hand results in a much weaker flow response (orange dashed line $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}|CC}$).

Figure 11.

Response of $v$ and $T$ due to forcing from various wall-normal regions. Response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | CC}$ due to forcing restricted to the core region (dashed orange curve), response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | OO}$ due to forcing restricted to the near-wall and outer region (dash-dotted blue curve), response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | CO}$ due to the covariance of the forcing between the two regions (dotted red curve). The three curves sum to the total flow response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}}$ (solid black line). The dashed and dotted lines in the inset show the flow response to forcing in the inner region, whose wall-normal extent is indicated by the grey shaded area.

It is also interesting to note that the response to forcing in the near-wall and outer regions alone ($\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}|OO}$) consistently overshoots the true flow statistics of $v$ and $T$. The covariance of the forcing between the two wall-normal regions results in damping (dotted red line $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}|CO}$) that adjusts the response to the correct amplitude in the outer region and beyond.

So far, the flow response, which peaks in the core region, has been attributed to non-local forcing in the layer that extends from $y=0.8$ down to the wall. This forcing region thus contains the critical layer of the Fourier mode $\boldsymbol {k}_G$ at $y \approx 0.53$ (horizontal line in figure 6), which is important to be effective at inducing a flow response. However, this region also contains the energetic near-wall turbulence that leads to a substantial near-wall forcing (see figure 6b,d). We now examine whether this near-wall turbulence contributes to the generation of internal gravity waves. To investigate this aspect, the forcing CSD is split again by wall-normal location, but this time with a boundary at $\{ y, y^{\prime } \} = 0.3$ and $1.7$. The resulting flow response is shown in the insets of figure 11, with the selected extent of the inner region indicated by the grey shaded area. The dashed and dotted curve represent the response to forcing where either one or both of $y$ and $y^{\prime }$ are located in the inner region and it is evident that the associated flow response is nearly zero. This behaviour is true as long as the divide of the CSD is at $y \leq 0.3$ and the maximum $y = 0.3$ is therefore taken as the boundary of the inner layer and shown in figure 11. The inner layer therefore represents a flow region with active turbulence, which includes the near-wall cycle and peak in turbulent kinetic energy production, but the nonlinear forcing in this region does not contribute to internal gravity waves, at least at $\boldsymbol {k}_G$.

In summary, the majority of the gravity wave is generated from forcing in the outer layer $0.3 < y < 0.8$ (red dotted line $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | CO}$ and blue dash-dotted curve $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | OO}$), which is approximately centred around the critical layer of the mode at $y \approx 0.53$.

5.2. Phase relation between response to velocity and temperature forcing

We next introduce a physics-based decomposition of the forcing, and examine how the resulting flow responses lead to localization in $y$. Specifically, instead of splitting the forcing CSD by wall-normal region as in § 5.1, we now split it by forcing contributions from the momentum equations, the temperature equations and their covariance. This partition of the forcing CSD results in three sub-matrices:

(5.4)\begin{equation} \hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k}} = \hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k}|\boldsymbol{uu}} + \hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k}|TT} + \hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k}|\boldsymbol{u}T}. \end{equation}

The subscript $\boldsymbol {u}$ or $T$ indicate which block matrices of $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k}}$ are non-zero for a given partition. For example, $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k}|TT}$ represents contributions from temperature forcing alone and only has one non-zero block. Analogously, $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k}|\boldsymbol {uu}}$ represents velocity forcing alone (first $3 \times 3$ blocks are non-zero) and $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k}|\boldsymbol {u}T}$ captures the covariance between velocity and temperature forcing.

The flow response to each sub-matrix of the forcing CSD is shown in figure 12 in terms of $s_{\boldsymbol {k} vv}$ and $s_{\boldsymbol {k} TT}$. The majority of the total flow response (black solid line) comes from the velocity forcing (blue dash-dotted line), while the contribution from the temperature forcing (orange dashed line) is significantly smaller. Interestingly, the flow response to the covariance between velocity and temperature forcing leads to negative contributions to the $v$ and $T$ statistics. These cancellations are required to localize the temperature response, as is evident from figure 12, and they limit the magnitude of the velocity and temperature fluctuations in the channel core. In the context of the resolvent bases discussed in § 4, these results indicate that the projection of the nonlinear velocity and temperature forcing onto the right singular vectors leads to different complex phases. These phases in turn translate to cancelling effects between the associated response modes, which leads to the localization of the gravity waves in $y$. It is also important to keep in mind from the previous section that the forcing in the outer region contributes most to the internal gravity waves. The observed destructive interference is largely due to the velocity and temperature forcing in this region as well.

Figure 12.

Response PSD of $v$ and $T$ due to forcing from various nonlinear terms. Response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | TT}$ due to temperature forcing alone (dashed orange curve), response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | \boldsymbol {uu}}$ due to velocity forcing alone (dash-dotted blue curve) and response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | \boldsymbol {u} T}$ due to covariance between velocity and temperature forcing (dotted red curve). The three curves sum to the total response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}}$ (solid black line).

5.3. Physical interpretation of localization

The throughout negative value of $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}|CO}$ in figure 11 and $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}|\boldsymbol {u}T}$ in figure 12 hint at distinct relative phase shifts between the flow response to forcing sub-blocks. This is perhaps not immediately obvious from the CSD itself and it is therefore instructive to decompose the forcing CSD into SPOD modes, which have a clear physical interpretation, and to study the associated flow response. A visual representation of this approach is given in the bottom right of figure 2. The forcing SPOD modes $\hat {\boldsymbol {\chi }}_{\boldsymbol {k}}$ are obtained from the eigenvalue problem

(5.5)\begin{equation} \hat{\boldsymbol{\mathsf{P}}}_{\boldsymbol{k}} \boldsymbol{\mathsf{W}} \hat{\boldsymbol{\chi}}_j = \lambda_j \hat{\boldsymbol{\chi}}_j, \end{equation}

where $\lambda _j$ denotes the associated eigenvalue that describes the energy contribution of each mode. The SPOD modes are orthonormal with respect to the energy inner product $(\hat {\boldsymbol {\chi }}_i, \hat {\boldsymbol {\chi }}_j)_E = \delta _{ij}$ and can be used to expand the solenoidal forcing at each $\boldsymbol {k}$ according to

(5.6)\begin{equation} \hat{\boldsymbol{f}}_{\boldsymbol{k}} = \sum_j \underbrace{(\hat{\boldsymbol{\chi}}_j, \hat{\boldsymbol{f}}_{\boldsymbol{k}} )_E}_{=\hat{a}_j} \hat{\boldsymbol{\chi}}_j. \end{equation}

The complex-valued expansion coefficients $\hat {a}_j$ are uncorrelated and can be related to the SPOD eigenvalues

(5.7)\begin{equation} \mathbb{E} [ \hat{a}_i \hat{a}_j^{{\ast}} ] = \lambda_i \delta_{ij}. \end{equation}

Interested readers may refer to Towne et al. (Reference Towne, Schmidt and Colonius2018) for further details on the SPOD.

Different from the standard approach, we are interested in the forcing SPOD modes not based on this eigenvalue but rather on the total energy of the associated flow response,

(5.8)\begin{equation} \lvert \hat{e}_j \rvert^2 = \lambda_j (\boldsymbol{\mathsf{R}} \hat{\boldsymbol{\chi}}_j, \boldsymbol{\mathsf{R}} \hat{\boldsymbol{\chi}}_j)_E, \end{equation}

since we are interested in energetic flow structures that arise from the forcing. The total energy of the flow response to each forcing SPOD mode is shown in figure 13, where the indices $j$ are ordered based on the SPOD eigenvalues. The decay of total energy is less pronounced than the typical decay of $\lambda _j$, but nonetheless provides an objective metric to select a SPOD mode to illustrate the physical mechanism that leads to the negative correlation coefficients. The following analysis will focus on the first SPOD mode $\hat {\boldsymbol {\chi }}_1$, which leads to the most energetic flow response, but it is important to point out that the same conclusions apply to all $j$ with substantial $\lvert \hat {e}_j \rvert$.

Figure 13.

Total energy of the flow response to forcing with the $j$th SPOD mode.

The spatial representation of the leading SPOD forcing mode and associated flow response is shown in figure 14. Each quantity is normalized by its maximum value, which is indicated above the figure. The mode represents a periodic structure in $x$ and $z$ (with periodicities $\lambda _x = \lambda _z = {\rm \pi}$) that advects downstream at the speed $c^+ = 21$. The mode shape is shown for a $yz$ cross-section of the channel. Also keep in mind that the $x$ and $z$ coordinate are interchangeable for this specific mode, since $k_x = k_z = 2$. The wall-normal velocity (line contours in figure 14(b), with positive contours drawn as solid and negative contours as dashed lines) and temperature forcing (colour contours) extend throughout the channel, with peaks in the outer and core regions (delineated by the horizontal lines). This lack of wall-normal localization in the forcing SPOD mode is consistent with the full forcing statistics (see figure 6).

Figure 14.

Spatial structure of the leading SPOD forcing mode $\hat {\boldsymbol {\chi }}_{1}$ (b) and associated flow response (a). In each figure, the contour lines indicate the normalized $v$ component of the velocity response and forcing, respectively, while the colour contours represent temperature. The contour lines denote $\{ -0.75, -0.5, \ldots, 0.75 \}$, with positive values shown as solid and negative values as dashed lines. The horizontal lines denote the core region of the channel.

The flow response to the leading SPOD mode on the other hand is clearly localized in the core region, as illustrated in figure 14(a). It is also apparent that the $v$ (contour lines) and $T$ (colour contours) flow response are shifted by about ${\rm \pi} / 2$ or, equivalently, quarter of a wavelength. This phase shift is consistent with the phase relation set by the linearized temperature equation and is commonly interpreted in the literature as additional evidence for the presence of internal gravity waves (see e.g. García-Villalba & del Álamo Reference García-Villalba and del Álamo2011).

We next give a physical interpretation of the negative response PSD contributions that result from the covariance of the forcing in the core and outer region ($\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}|CO}$ in figure 11). Analogous to the partitioning of $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k}}$ in § 5.1, we split the forcing SPOD mode into wall-normal sub-vectors

(5.9)\begin{equation} \hat{\boldsymbol{\chi}}_{1} = \hat{\boldsymbol{\chi}}_{1 | C} + \hat{\boldsymbol{\chi}}_{1 | O}. \end{equation}

As before, the subscript $C$ denotes the vector that contains non-zero entries at all $y$ locations in the core region, while the subscript $O$ denotes the vector with non-zero entries in the near-wall and outer regions. Note that unlike $\hat {\boldsymbol{\mathsf{P}}}_{\boldsymbol {k}}$, the SPOD modes are linear in $\boldsymbol {f}$ so that there is no cross-term between the two regions. We can now study the flow response to each subset of the forcing independently,

(5.10)\begin{equation} \boldsymbol{\mathsf{R}} \hat{\boldsymbol{\chi}}_{1} = \boldsymbol{\mathsf{R}} \hat{\boldsymbol{\chi}}_{1 | C} + \boldsymbol{\mathsf{R}} \hat{\boldsymbol{\chi}}_{1 | O}, \end{equation}

and the corresponding spatial structures are shown in figure 15. In both cases, the response is localized in the channel core and the velocity and temperature responses are shifted by ${\rm \pi} / 2$ relative to each other. As anticipated from figure 11, the response to forcing in the near-wall and outer regions is appreciably stronger than that to forcing in the core region, and dominates the overall response. The spatial structures of the two responses have a distinct spatial arrangement relative to each other, as becomes apparent by comparing the flow structure along the vertical orange line, which marks $z = 1.0$. The wall-normal velocity response (black contour lines) to $\hat {\boldsymbol {\chi }}_{1 | C}$ reaches its minimum close to $z = 1.0$, while the corresponding response to $\hat {\boldsymbol {\chi }}_{1 | O}$ reaches its maximum. In other words, the two flow structures are approximately out of phase and their pointwise products are negative valued. The same comment applies to the temperature response as well. The products of such cross-terms make up $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}|CO}$ and illustrate that the negative covariance between forcing in different wall-normal regions is due to relative spatial shifts in the corresponding responses. Since the covariance $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}|CO}$ is a product between a large (e.g. $\boldsymbol{\mathsf{R}} \hat {\boldsymbol {\chi }}_{1 | O}$) and a small term (e.g. $\boldsymbol{\mathsf{R}} \hat {\boldsymbol {\chi }}_{1 | C}$), its magnitude is smaller than $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}|OO}$, but larger than $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}|CC}$.

Figure 15.

Wall-normal velocity (black lines) and temperature (colour contours) response due to forcing restricted to the near-wall and outer regions (a) and core region (b), respectively. The contour levels are as in figure 14.

Finally, we illustrate the flow response to the covariance of velocity and temperature forcing, which generates negative contributions to the response PSD in figure 16 (red dotted line $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | \boldsymbol {u} T}$). To this end, we split the leading forcing SPOD mode into velocity and temperature components

(5.11)\begin{equation} \hat{\boldsymbol{\chi}}_{1} = \hat{\boldsymbol{\chi}}_{1 | \boldsymbol{u}} + \hat{\boldsymbol{\chi}}_{1 | T}, \end{equation}

where, for example, $\hat {\boldsymbol {\chi }}_{1 | \boldsymbol {u}}$ contains all the velocity forcing entries. The response to each subset of the forcing can then be studied independently,

(5.12)\begin{equation} \boldsymbol{\mathsf{R}} \hat{\boldsymbol{\chi}}_1 = \boldsymbol{\mathsf{R}} \hat{\boldsymbol{\chi}}_{1 | \boldsymbol{u}} + \boldsymbol{\mathsf{R}} \hat{\boldsymbol{\chi}}_{1 | T}, \end{equation}

and the corresponding spatial structures are shown in figure 16. It is important to recall that the sum of the two sub-figures recovers the total flow response shown in figure 14(a).

Figure 16.

Wall-normal velocity (black lines) and temperature (colour contours) response due to velocity forcing (a) and temperature forcing (b). The contour levels are as in figure 14.

We first discuss the shared features in both responses and then comment on the relative phase differences. For each flow response, the velocity and temperature have a relative phase shift of ${\rm \pi} / 2$. The robustness of this phase difference suggests that it depends only weakly on the details of the forcing and is imprinted by the linear dynamics. Both flow responses further have local maxima in the channel core, but their level of localization varies. For example, the temperature responses (colour contours) extend well into the outer region, while the $v$ responses (black contour lines) do not. The overall temperature response (figure 14a) is also more localized, which suggests that the relative phase between the sub-vector responses leads to cancellations.

To explore this aspect, we compare the flow responses across the figures and use the reference location $z = 1$, marked by the orange vertical line. The two wall-normal velocity responses are both localized in the channel core and are almost out of phase, so that their pointwise products are mostly negative. The phase relation of the temperature response is more complex and depends on the wall-normal location. The two temperature responses are out of phase in the outer region and, thus, cancel out and localize the overall temperature response in the channel core. Within the core, the phase shift between the two temperature responses approaches ${\rm \pi} / 2$ towards the channel centre, and the overall response localizes similarly to figure 16(a), which is dominant. Pointwise products between quantities like $\boldsymbol{\mathsf{R}} \hat {\boldsymbol {\chi }}_{1 | \boldsymbol {u}}$ and $\boldsymbol{\mathsf{R}} \hat {\boldsymbol {\chi }}_{1 | T}$ make up $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}|uT}$ and the extended spatial regions where this product is negative (i.e. where the two responses are out of phase) generate the negative contributions to the response PSD. A comparison between the overall and component-wise responses suggests that robust phase relations are necessary to localize the overall flow response in the core region, especially the temperature field.

5.4. Behaviour at higher Richardson number

The analysis of the nonlinear dynamics has so far focused on the weakly stratified flow R60 (${Ri}_{\tau } \approx 60$, ${Re}_{\tau } \approx 180$). The present section explores whether the three-layer flow structure and the destructive interference that localize the flow response in $y$ persist at higher stratification levels. To this end, we analyse configuration R120 (${Ri}_{\tau } \approx 120$, ${Re}_{\tau } \approx 180$), which in preliminary simulations was identified to be near the stratification limit for sustaining a fully turbulent flow at the given Reynolds number. Narrow laminar patches typical of strongly stratified channel flows appear in the near-wall region at this Richardson number, but no low-frequency oscillations are observed in the time series of planar-averaged quantities, indicating that the domain is sufficiently large relative to the size of the patches (see García-Villalba & del Álamo Reference García-Villalba and del Álamo2011 for an in-depth discussion). It is also important to emphasize that the flow is fully turbulent beyond the near-wall region and, in particular, in the channel core.

The analysis follows the approach outlined in §§ 3, 4, 5.1 and 5.2, but only the most relevant results are shown here for conciseness. In a first step, a pair of suitable streamwise and spanwise wavenumbers is identified from the time-averaged $v$ and $T$ PSDs. Again, large streamwise and spanwise scales contribute most to the velocity and temperature fluctuations in the channel core, and are suitable candidates. The scale $\boldsymbol {\xi }_G = (k_x = 2, k_z = 2)^{\top }$ studied in the previous sections lies within this energetic spectral region and will serve as a representative example also in the following analysis to enable meaningful comparisons with case R60. The temporal PSDs of $v$ and $T$ at $\boldsymbol {\xi }_G$ are shown in figure 17, along with reference data from cases R0 and R60. Analogous to case R60, the structures in the channel core advect more slowly than the mean flow and it is clear that the offset from the mean increases with stratification. The energy content further clusters around the slower wave speed of the empirical dispersion relation for internal gravity waves (dark blue triangle), but no imprint of the faster travelling solution is observed. The most energetic wave speed in the temperature response occurs at $c^+ \approx 22.4$, and we will subsequently analyse the mode $\boldsymbol {k}_G = (k_x = 2, k_z = 2, c^+ = 22.4)^{\top }$ as an example for internal gravity waves in configuration R120.

Figure 17.

Temporal PSD of the Fourier mode $\boldsymbol {\xi }_{G}$. The PSDs in (a) and (b) are normalized by their maximum value, which is reported above each figure in order {R0 (light blue), R60 (medium blue), R120 (dark blue)}. The contour lines label $\boldsymbol {s}_{\boldsymbol {k}} / (\max \boldsymbol {s}_{\boldsymbol {k}}) = \{ 0.25, 0.5, 0.75 \}$, the dashed lines indicate the mean-velocity profiles and the dark blue triangles denote the wave speed of the gravity waves according to the empirical relation of Lloyd et al. (Reference Lloyd, Dorrell and Caulfield2022) for case R120. The green vertical line denotes $c^+ = 22.4$, which will be analysed subsequently, and the dotted horizontal line marks the associated critical-layer height ($y \approx 0.48$).

Similar to the earlier results at R60, the flow response for R120 is localized in spectral space and in $y$, while the nonlinear forcing is not similarly localized (not shown). A detailed analysis of the linear dynamics for case R120 is beyond the scope of this section; however, we note that the largest linear energy amplification is again highly selective in $c$. Moreover, the peak wave speed of the temperature PSD at $c^+ \approx 22.4$ coincides with the location of maximum energy amplification, which occurs at $c^+ \approx 22.1$. These observations suggest that the linear dynamics localize the flow response in spectral space at higher stratification levels as well.

We now turn our attention to the nonlinear dynamics and localization in the wall-normal direction. In a first step, the analysis of § 5.1 is repeated to investigate if the nonlinear forcing of flow R120 exhibits the same three-layer structure. Figure 18 shows the response to wall-normal sub-blocks of the forcing CSD, as defined earlier in (5.2) and (5.3). The inset confirms that an inner layer, whose forcing does not contribute significantly to the internal gravity waves (dashed and dotted lines), exists under stronger stratification as well. The wall-normal extent of the inner layer depends on the Richardson number and decreases with stratification: for case R60, it extended from the wall to $y = 0.3$, while in the present configuration R120 it only extends to $y = 0.2$ (indicated by the grey shaded area). The majority of the internal gravity wave is generated from forcing in the outer region (blue dash-dotted curve $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | OO}$), which is approximately centred around the critical layer of the mode ($y \approx 0.48$, see figure 17). The nonlinear forcing in the core region generates a weak flow response ($\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | CC}$), but the negative contributions of $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | CO}$ (response to covariance between forcing in the two regions) are required to limit the wave amplitude. These observations are consistent with flow R60 and confirm that the three-layer structure persists at higher ${Ri}$.

Figure 18.

Response of $v$ and $T$ due to forcing from various wall-normal regions at ${Ri}_{\tau } = 120$. Response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | CC}$ due to forcing restricted to the core region (dashed orange curve), response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | OO}$ due to forcing restricted to the outer region (dash-dotted blue curve) and response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | CO}$ due to the covariance of the forcing between the two regions (dotted red curve). The inset shows that forcing from the inner region does not contribute to the flow response. The coloured curves sum to the total flow response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}}$ (solid black line).

Finally, we explore if destructive interference between the response to velocity and temperature forcing is still required to localize the flow response at stronger stratification. Figure 19 shows the flow response to velocity and temperature sub-blocks of the forcing CSD, according to (5.4). With regards to the wall-normal velocity response, $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | \boldsymbol {u} T}$ is close to zero throughout the channel, which indicates that the response to velocity and to temperature forcing are approximately ${\rm \pi} / 2$ out of phase and do not interact. This is different from the destructive interference that limited the $v$ amplitude in case R60. The features of the temperature response on the other hand are very similar to the less stratified case. In particular, it is apparent that the cancellations persist and are required to limit the extent of the gravity waves to the channel core even at higher stratification levels.

Figure 19.

Response PSD of $v$ and $T$ due to forcing from various nonlinear terms at ${Ri}_{\tau } = 120$. Response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | TT}$ due to temperature forcing alone (dashed orange curve), response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | \boldsymbol {uu}}$ due to velocity forcing alone (dash-dotted blue curve) and response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k} | \boldsymbol {u} T}$ due to covariance between velocity and temperature forcing (dotted red curve). The three curves sum to the total response $\hat {\boldsymbol{\mathsf{S}}}_{\boldsymbol {k}}$ (solid black line).