2.1. Spectral proper orthogonal decomposition

In the following, we provide an outline of a specific procedure of computing SPOD based on Welch's method (Welch Reference Welch1967) and emphasise aspects that are important in the context of data reconstruction. Refer to the work of Towne et al. (Reference Towne, Schmidt and Colonius2018) for details of the derivation and mathematical properties, and Schmidt & Colonius (Reference Schmidt and Colonius2020) for a practical introduction to the method.

Given a fluctuating flow field $\boldsymbol {q}_{i}=\boldsymbol {q}(t_i)$, where $i=1,\ldots ,{n_t}$, which is obtained by subtracting the temporal mean $\bar {\boldsymbol {q}}$ from each snapshot of the data, we start by constructing a snapshot matrix

(2.1)\begin{equation} \boldsymbol{\mathsf{Q}}= {\left[{ \boldsymbol{q}_1, \boldsymbol{q}_2, \ldots, \boldsymbol{q}_{n_t} }\right]}. \end{equation}

Note that multi-dimensional data are cast into the form of a vector $\boldsymbol {q}_{i}$ of length $n$, corresponding to the number of variables times the number of grid points. The instantaneous energy of each time instant, or snapshot, is expressed in terms of a spatial inner product

(2.2)\begin{equation} \|\boldsymbol{q}\|_x^{2}=\left\langle\boldsymbol{q},\boldsymbol{q} \right\rangle_x = \int_{\varOmega} \boldsymbol{q}^{*}(x,t)\boldsymbol{W}(x)\boldsymbol{q}(x,t) \,{\textrm{d}\kern0.7pt x}, \end{equation}

where $\boldsymbol{W}$ is a positive-definite Hermitian matrix that accounts for the component-wise weights, $\varOmega$ the spatial domain of interest and $(.)^{*}$ denotes the complex conjugate. The common form of space-only POD is obtained as the eigendecomposition of $\boldsymbol{\mathsf{Q}} \boldsymbol{\mathsf{Q}}^{*} \boldsymbol{\mathsf{W}}$ and yields modes that are optimal in terms of (2.2). The SPOD, however, specialises POD for statistically stationary processes and seeks modes that are optimal in terms of the space–time inner product

(2.3)\begin{equation} \|\boldsymbol{q}\|_{x,t}^{2}=\left\langle\boldsymbol{q},\boldsymbol{q} \right\rangle_{x,t} = \int_{-\infty}^{\infty} \int_{\varOmega} \boldsymbol{q}^{*}(x,t)\boldsymbol{W}(x)\boldsymbol{q}(x,t)\, \mathrm{d}\kern0.7pt x\, \mathrm{d} t. \end{equation}

For statistically stationary data, it is natural to proceed in the frequency domain and solve the POD eigenvalue problem for the Fourier transformed two-point space–time correlation matrix, that is, the CSD matrix. To estimate the CSD, the data are segmented into $n_{ blk}$ overlapping blocks with $n_{ fft}$ snapshots in each of them, as

(2.4)\begin{equation} {\boldsymbol{\mathsf{Q}}}^{(k)}={\left[{\boldsymbol{q}_1^{(k)}, \boldsymbol{q}_2^{(k)}, \ldots, \boldsymbol{q}_{n_{ fft}}^{(k)} }\right]}. \end{equation}

If the blocks overlap by $n_{ ovlp}$ snapshots, the $j$-th column in the $k$-th block is given by

(2.5)\begin{equation} \boldsymbol{q}_{j}^{(k)}=\boldsymbol{q}_{j+(k-1)(n_{ fft}-n_{ ovlp})+1}. \end{equation}

Each block is considered as a statistically independent realisation of the flow under the ergodic hypothesis. The motive behind the segmentation of data is to increase the number of ensemble members. In practice, a windowing function is applied to each block to reduce spectral leakage. In this study, we use the symmetric Hamming window

(2.6)\begin{equation} w(i+1)=0.54-0.46 \cos{{\left({\frac{2 {\rm \pi}i}{n_{ fft} -1} }\right)}} \quad\text{for}\ i=0,1, \ldots, n_{ fft}-1. \end{equation}

Following best practices established by Harris (Reference Harris1978), we only apply windowing for overlapping blocks to avoid excessive loss of information at the boundaries, i.e. if $n_{ ovlp} \neq 0$. Subsequently, the weighted temporal discrete Fourier transform,

(2.7)\begin{equation} \hat{\boldsymbol{q}}_{j}^{(k)}=\mathcal{F}{\left\{{w(\,j)\boldsymbol{q}_{j}^{(k)}}\right\}}, \end{equation}

is performed on each windowed block to obtain the Fourier-transformed data matrix

(2.8)\begin{equation} \hat{\boldsymbol{\mathsf{Q}}}^{(k)}={\left[{\hat{\boldsymbol{q}}_1^{(k)}, \hat{\boldsymbol{q}}_2^{(k)},\ldots, \hat{\boldsymbol{q}}_{n_{ fft}}^{(k)} }\right]}, \end{equation}

where $\hat {\boldsymbol {q}}_i^{(k)}$ denotes the $k$-th Fourier realisation at the $i$-th discrete frequency. Next, we reorganise the data by frequency. The matrix containing all realisations of the Fourier transform at the $l$-th frequency reads

(2.9)\begin{equation} \hat{\boldsymbol{\mathsf{Q}}}_{l}={\left[{\hat{\boldsymbol{q}}_{l}^{(1)}, \hat{\boldsymbol{q}}_{l}^{(2)},\ldots, \hat{\boldsymbol{q}}_{l}^{(n_{ blk})} }\right]}. \end{equation}

From this form, the SPOD modes, $\boldsymbol {\varPhi }$, and associated energies, $\lambda$, can be computed as the eigenvectors and eigenvalues of the CSD matrix $\boldsymbol{\mathsf{S}}_l= \hat{\boldsymbol{\mathsf{Q}}}_{l} \hat{\boldsymbol{\mathsf{Q}}}_{l}^{*}$. In practice, the number of spatial degrees of freedom, $n$, is often much larger than number of realisations. In this case, it is more economical to solve the analogous eigenvalue problem

(2.10)\begin{equation} \frac{1}{n_{ blk}}\hat{\boldsymbol{\mathsf{Q}}}_{l}^{*}\boldsymbol{\mathsf{W}} \hat{\boldsymbol{\mathsf{Q}}}_{l} \boldsymbol{\varPsi}_{l}=\boldsymbol{\varPsi}_{l} \boldsymbol{\varLambda}_{l} \end{equation}

for the coefficients $\boldsymbol {\psi }$ that expand the SPOD modes in terms of the Fourier realisations. In terms of the column matrix $\boldsymbol {\varPsi }_{l}=[\psi _l^{(1)}, \psi _l^{(2)}, \ldots, \psi _l^{(n_{ blk})}]$, the SPOD modes at the $l$-th frequency are recovered as

(2.11)\begin{equation} \boldsymbol{\varPhi}_{l} = \frac{1}{\sqrt{n_{blk}}}\hat{\boldsymbol{\mathsf{Q}}}_{l} \boldsymbol{\varPsi}_{l} \boldsymbol{\varLambda}_{l}^{{-}1/2}. \end{equation}

The matrices $\boldsymbol {\varLambda }_{l}=\text {diag} ( \lambda _{l}^{(1)}, \lambda _{l}^{(2)}, \ldots , \lambda _{l}^{(n_{ blk})} )$, where by convention $\lambda _{l}^{(1)} \ge \lambda _{l}^{(2)} \ge \cdots \ge \lambda _{l}^{(n_{ blk})}$, and $\boldsymbol {\varPhi }_{l}=[ \boldsymbol {\phi }_{l}^{(1)}, \boldsymbol {\phi }_{l}^{(2)}, \ldots , \boldsymbol {\phi }_{l}^{(n_{ blk})} ]$ contain the SPOD energies and modes, respectively. By construction, the SPOD modes are orthogonal in the space–time inner product (2.3). At any given frequency, the modes are also orthogonal in the spatial inner product (2.2).

2.2. Data reconstruction

In § 2.2.1, we show how the data can be reconstructed in the frequency domain, that is, the inversion of the SPOD. An alternative approach based on (oblique) projection in the time domain is presented in § 2.2.2. Whether one approach or the other is preferred depends on the specific application. Detailed discussions for each application under consideration in this work can be found in § 3. We will use the term ‘frequency domain’ if the expansion coefficients are computed using the inversion of the SPOD problem, (2.13), and ‘time domain’ if oblique projection, (2.19), is used.

2.2.1. Reconstruction in the frequency domain

The common factor of the different applications of SPOD considered in this study is that they require truncation or re-weighting of the SPOD basis. In practice, this is achieved by modifying the expansion coefficients. The original realisations of the Fourier transform at each frequency can be reconstructed as

(2.12)\begin{equation} \hat{\boldsymbol{\mathsf{Q}}}_{l}= \boldsymbol{\varPhi}_l \boldsymbol{\mathsf{A}}_l, \end{equation}

where $\boldsymbol{\mathsf{A}}_l$ is the matrix of expansion coefficients:

(2.13)\begin{equation} \boldsymbol{\mathsf{A}}_{l} =\sqrt{n_{ blk}} \boldsymbol{\varLambda}^{1/2}_{l} \boldsymbol{\varPsi}^{*}_{l} = \boldsymbol{\varPhi}_l^{*} \boldsymbol{\mathsf{W}} \hat{\boldsymbol{\mathsf{Q}}}_{l}. \end{equation}

Equation (2.13) shows that the expansion coefficients can either be saved during the computation of SPOD or be recovered later by projecting the Fourier realisations onto the modes. In the following, we omit the frequency index $l$ with the understanding that the SPOD eigenvalue problem is solved at each frequency separately. From (2.12), it can be inferred that each column of the matrix

(2.14) \begin{equation} \boldsymbol{\mathsf{A}} = \left[\begin{array}{@{}cccc@{}} a_{11} & a_{12} & \cdots & a_{1 n_{ blk}} \\ a_{21} & a_{22} & \cdots & a_{2 n_{ blk}} \\ \vdots & \vdots & \ddots & \vdots \\ a_{n_{ blk} 1} & a_{n_{ blk} 2} & \cdots & a_{n_{blk} n_{blk}} \end{array}\right], \end{equation}

contains the expansion coefficients that allow for the reconstruction of a specific Fourier realisation from the SPOD modes. Vice versa, the coefficients contained in each row of $\boldsymbol{\mathsf{A}}$ can be used to expand a specific SPOD mode in terms of the Fourier realisations. This can most easily be seen by rewriting (2.12) as $\boldsymbol{\varPhi}_l = ({1}/{n_{ blk}})\hat{\boldsymbol{\mathsf{Q}}}_{l}\boldsymbol{\mathsf{A}}_l^{*}\boldsymbol{\varLambda}^{-1}_l$. The Fourier-transformed data of the $k$-th block can be reconstructed as

(2.15)\begin{equation} \hat{\boldsymbol{\mathsf{Q}}}^{(k)}= {\left[{ {\left({\sum_{i} a_{ik} \boldsymbol{\phi}^{(i)}}\right)}_{l=1}, {\left({\sum_{i} a_{ik} \boldsymbol{\phi}^{(i)}}\right)}_{l=2}, \ldots, {\left({\sum_{i} a_{i k} \boldsymbol{\phi}^{(i)}}\right)}_{l=n_{ fft}}}\right]}. \end{equation}

The original data in the $k$-th blocks ${\boldsymbol{\mathsf{Q}}}^{(k)}$ can now be recovered using the inverse (weighted) Fourier transform

(2.16)\begin{equation} {\boldsymbol{q}}_{j}^{(k)}=\frac{1}{w(\,j)}\mathcal{F}^{{-}1}{\left\{{\hat{\boldsymbol{q}}_{j}^{(k)}}\right\}}. \end{equation}

Reconstructing the time series from the reconstructed data segments concludes the inversion of the SPOD.

A schematic of the windowing and blocking strategy is shown in figure 1. The use of overlapping blocks leads to an ambiguity in the reconstruction as the $i$-th snapshot can either be obtained from the $k$-th block as ${\boldsymbol {q}}^{(k)}_{j}$, or from the $(k+1)$-th block as ${\boldsymbol {q}}^{(k+1)}_{j+n_{ ovlp}- n_{ fft}}$. Different possibilities to remove this ambiguity are described in Appendix A. Based on this discussion, snapshots are reconstructed as averages of two reconstructions from overlapping blocks, weighted by the relative value of their windowing function. Partial reconstructions in the frequency domain are readily achieved by zeroing the expansion coefficients of specific modes prior to applying the inverse Fourier transform.

Figure 1.

Schematic representation of overlapping blocks, Hamming window and the SPOD parameters such as $n_t$, $n_{{fft}}$, $n_{{ovlp}}$ and $n_{{blk}}$. The left and right blocks are denoted using blue and red lines, respectively. The vertical line corresponds to the snapshot number 210, and the blue and red circles indicate the corresponding value of the window function.

2.2.2. Reconstruction in the time domain

As an alternative to the reconstruction in the frequency domain, we present in the following a projection-based approach in the time domain. This approach is computationally efficient, and has the advantage that it can be applied to new data that was not used to compute SPOD and to individual snapshots. However, the time-domain reconstruction does not leverage the orthogonality of the SPOD modes in the space–time inner product. Instead, it is based on an oblique projection of the data onto the modal basis. We start by representing the data as a linear combination of the SPOD modes as

(2.17)\begin{equation} \boldsymbol{\mathsf{Q}}\approx \tilde{\boldsymbol{\varPhi}} \tilde{\boldsymbol{\mathsf{A}}}. \end{equation}

The matrix $\tilde{\boldsymbol{\varPhi}}$ contains the basis of SPOD modes at all frequencies. Arranging the basis vectors by frequency first, we write

(2.18)\begin{equation} \tilde{\boldsymbol{\varPhi}}= {\left[{\boldsymbol{{\phi}}_{1}^{(1)}, \boldsymbol{{\phi}}_{1}^{(2)}, \ldots, \boldsymbol{{\phi}}_{1}^{(n_{ blk})}, \boldsymbol{{\phi}}_{2}^{(1)}, \boldsymbol{{\phi}}_{2}^{(2)}, \ldots, \boldsymbol{{\phi}}_{2}^{(n_{ blk})}, \ldots, \boldsymbol{{\phi}}_{n_{ fft}}^{(1)}, \boldsymbol{{\phi}}_{n_{ fft}}^{(2)}, \ldots, \boldsymbol{{\phi}}_{n_{ fft}}^{(n_{ blk})} }\right]}. \end{equation}

Assuming that $\tilde{\boldsymbol{\varPhi}}$ has full column rank, the matrix of expansion coefficient is obtained from the weighted oblique projection

(2.19)\begin{equation} \tilde{\boldsymbol{\mathsf{A}}} = {\left({\tilde{\boldsymbol{\varPhi}}^{*} \boldsymbol{\mathsf{W}} \tilde{\boldsymbol{\varPhi}}}\right)}^{{-}1} \tilde{\boldsymbol{\varPhi}}^{*} \boldsymbol{\mathsf{W}} \boldsymbol{\mathsf{Q}}. \end{equation}

The oblique projection is required as SPOD modes at different frequencies are not orthogonal in the purely spatial inner product, $\langle \cdot ,\cdot \rangle _x$, defined in (2.2). We furthermore use a weighted oblique projection based on the weight matrix $\boldsymbol{\mathsf{W}}$ to guarantee compatibility with this inner product. Using the oblique projection, a single snapshot $\boldsymbol {q}=\boldsymbol {q}(\boldsymbol {x},t)$ is represented in the SPOD basis as

(2.20)\begin{equation} \tilde{\boldsymbol{q}} = \tilde{\boldsymbol{\varPhi}} {\left({\tilde{\boldsymbol{\varPhi}}^{*} \boldsymbol{\mathsf{W}} \tilde{\boldsymbol{\varPhi}}}\right)}^{{-}1} \tilde{\boldsymbol{\varPhi}}^{*} \boldsymbol{\mathsf{W}} \boldsymbol{q}, \end{equation}

and the entire data are recovered as

(2.21)\begin{equation} \tilde{\boldsymbol{\mathsf{Q}}} = \tilde{\boldsymbol{\varPhi}} \tilde{\boldsymbol{\mathsf{A}}}. \end{equation}

In the case where $\tilde{\boldsymbol{\varPhi}}$ is rank-deficient or ill-conditioned, $\tilde{\boldsymbol{\varPhi}}^{*} \boldsymbol{\mathsf{W}} \tilde{\boldsymbol{\varPhi}}$ is not invertible. For a general rank-$r$ matrix, we perform the symmetric eigenvalue decomposition

(2.22)\begin{equation} \tilde{\boldsymbol{\varPhi}}^{*} \boldsymbol{\mathsf{W}} \tilde{\boldsymbol{\varPhi}} = \boldsymbol{\mathsf{U}} \boldsymbol{\mathsf{D}} \boldsymbol{\mathsf{U}}^{*}, \quad\text{with}\ \boldsymbol{\mathsf{U}}=\left[ \boldsymbol{\mathsf{U}}_1 \; \boldsymbol{\mathsf{U}}_2\right],\; \boldsymbol{\mathsf{D}}=\left[\begin{array}{@{}cc@{}} \boldsymbol{\mathsf{D}}_1 & \boldsymbol{0} \\ \boldsymbol{0} & \boldsymbol{0}\end{array}\right], \end{equation}

where $\boldsymbol{\mathsf{D}}_1=\textrm {diag}({\mathsf{d}}_1,{\mathsf{d}}_2, \ldots , {\mathsf{d}}_r)$ with ${\mathsf{d}}_1\geq {\mathsf{d}}_2\geq \cdots \geq {\mathsf{d}}_r>0$ is the diagonal matrix of (numerically) non-zero eigenvalues and $\boldsymbol{\mathsf{U}}_1$ is the corresponding matrix of orthonormal eigenvectors. In some applications, we desire a more aggressive truncation to rank $k< r$. For full-rank reconstructions, we use a truncation threshold of ${d_k}/{d_1} = 10^{-6}$ in this work. Denoted by

(2.23)\begin{equation} \tilde{\boldsymbol{\mathsf{A}}}_{\{k\}} = \boldsymbol{\mathsf{U}}_{\{k\}} \boldsymbol{\mathsf{D}}_{\{k\}}^{{-}1} \boldsymbol{\mathsf{U}}_{\{k\}}^{*} \tilde{\boldsymbol{\varPhi}}^{*} \boldsymbol{\mathsf{W}} \boldsymbol{\mathsf{Q}}, \end{equation}

is the rank-$k$ approximation of $\tilde {\boldsymbol{\mathsf{A}}}$, where $\boldsymbol{\mathsf{D}}_{\{k\}}=\textrm {diag}({\mathsf{d}}_1,{\mathsf{d}}_2, \ldots , {\mathsf{d}}_k)$ and $\boldsymbol{\mathsf{U}}_{\{k\}}=[{\mathsf{u}}_1,{\mathsf{u}}_2, \ldots , {\mathsf{u}}_k]$. In the truncated basis, $\boldsymbol{\mathsf{U}}_{\{k\}} \boldsymbol{\mathsf{D}}_{\{k\}}^{-1} \boldsymbol{\mathsf{U}}_{\{k\}}^{*}$ approximates ${\left ({\tilde{\boldsymbol{\varPhi}}^{*} \boldsymbol{\mathsf{W}} \tilde{\boldsymbol{\varPhi}}}\right )}^{-1}$. In the following, we demonstrate how the above and other truncation and partial reconstruction strategies can be used to achieve a number of objectives in the processing of flow data.

3.1. Low-dimensional flow-field reconstruction

Since SPOD seeks an optimal series expansion for each frequency, the choice of what eigenpairs to include in a low-dimensional reconstruction is not obvious. Here we first discuss the most elementary way of truncation based on the frequency-wise optimality property, that is, a certain number of modes is retained at each frequency. We refer to this as a $n_{modes} \times n_{freq}$-mode reconstruction, where $n_{modes}$ is the number of modes retained at each frequency, and $n_{freq} = {n_{fft}}/{2}+1$ is the number of positive frequencies, including zero. If all modes are linearly independent, then the overall rank of the reconstructions is given by the total number of basis vectors, $n_{modes}n_{freq}$.

Following the discussion in § 2, we present two means of obtaining an SPOD-based low-dimensional reconstruction:

1. (i) in the frequency domain (see § 2.2.1) using (2.16); and

2. (ii) in the time domain (see § 2.2.2) using (2.20).

The frequency-domain approach directly follows from the mathematical definition of SPOD, and was previously used by Citriniti & George (Reference Citriniti and George2000), Jung et al. (Reference Jung, Gamard and George2004), Johansson & George (Reference Johansson and George2006b) and Tinney et al. (Reference Tinney, Glauser and Ukeiley2008a). The time-domain approach can be viewed as the most general approach that can be applied to any given modal basis. It is not specific to SPOD, but commonly used for low-order modelling.

In the following, we first compare different low-dimensional reconstructions in terms of their block-wise and snapshot-wise energy in figure 4. It follows from (2.3), that the energy of a single block is

(3.1)\begin{equation} \|\boldsymbol{q}\|_{x,t}^{2} = \left\langle\boldsymbol{q},\boldsymbol{q} \right\rangle_{x,t} = \int_{\Delta T} \int_{\varOmega} \boldsymbol{q}^{*}(x',t)\boldsymbol{W}(x')\boldsymbol{q}(x',t) \,\mathrm{d}\kern0.7pt x'\, \mathrm{d} t, \end{equation}

where $\Delta T = [t_{1+(k-1)(n_{ fft}-n_{ ovlp})},t_{{n_{ fft}}+(k-1)(n_{ fft}-n_{ ovlp})}]$ is the time interval of the $k$-th block. The spatial norm (2.2) measures the energy present in each snapshot. Both the block-wise and snapshot-wise pressure norms are computed for both reconstruction approaches. The evolution of the space–time norm is shown for the entire database in figure 4($a$,$c$). For the spatial norm, we focus on the first 768 snapshots in figure 4($b$,$d$). This segment corresponds to five blocks and exhibits dynamics that is representative of the rest of the data.

Figure 4.

Low-dimensional reconstruction of the jet data: frequency-domain reconstruction ($a$,$b$), and time-domain reconstruction ($c$,$d$) in terms of the space–time norm ($a$,$c$) and the spatial norm ($b$,$d$). The original data (blue lines), shown for reference, are compared with the full reconstructions using all modes, and reconstructions using 10 $\times$ 129, 3 $\times$ 129 and 1 $\times$ 129 modes. Summed SPOD mode energies are shown as dashed lines. Vertical dotted blue and red lines in ($b$,$d$) indicate the left and right blocks in the reconstruction (see figure 1).

Low-dimensional reconstructions using $1\times 129$, $3\times 129$, $10\times 129$ modes and the reconstruction using all modes are presented in figure 4. The dimension of the modal bases directly reflects their ability to capture the pressure norms of the data. The full-dimensional reconstructions in the frequency and time domain recover the data completely. Notably, the dynamics in space–time norm is accurately captured, even by the $1\times 129$-mode reconstruction. For a fixed number of modes, the time domain approach captures more energy and provides a better approximation of the data than the frequency-domain approach. Take as an example the $10 \times 129$ basis: the time-domain reconstruction accurately approximates for the full data (figure 4$c$,$d$), which is notably underpredicted by frequency-domain reconstruction (figure 4$a$,$b$). This difference can be understood by considering the SPOD energy content of the reconstruction. The dashed lines in figure 4($a$,$b$) denote this energy, which is given by the sum of the first $n_{ modes}$ eigenvalues over all frequencies. As expected, the space–time and spatial norm of the different reconstructions fluctuate about the sum of the eigenvalues. Higher energies are obtained by the time-domain reconstruction in figure 4($c$,$d$) as the modal expansion coefficients obtained via oblique projection are not bound to specific frequencies. In what follows, we will see again and again that this flexibility of the expansion coefficients of the time-domain approach leads to an overall better reconstruction. This additional degree of freedom can be leveraged to obtain an accurate reconstruction of the flow dynamics. It is, in fact, the optimality property of the oblique projection, (2.20), that guarantees that the time-domain approach yields the best possible approximation in a least-square sense. For example, the 1 $\times$ 129 time-domain reconstruction seen in figure 4($d$) is sufficient to capture the dynamics of the original data accurately. From figure 4($b$), it can be seen that the frequency-domain reconstruction significantly overpredicts the pressure norm during the first 32 snapshots. This effect only occurs for the two outermost blocks, which do not posses neighbouring blocks in one direction. In Appendix A (figure 20), we show by comparison with a rectangular window that this error is a result of the Hamming window. The presence of the windowing effect in the first and last blocks is equally reflected in the space–time norm, see figure 4($a$).

Figure 5 demonstrates that the frequency-domain approach accurately recovers the mode energies given by the SPOD eigenvalues. By adding the residual energy contained in the truncated eigenvalues, both the space–time norm (figure 5$a$) and the spatial norm (figure 5$b$) can be collapsed to the total energy. The remaining differences are largely due to the windowing effect.

Figure 5.

Low dimensional reconstruction in the frequency-domain with truncation correction: ($a$) space–time norm; ($b$) spatial norm. Panels ($a$,$b$) correspond to figure 4($a$,$b$), respectively, but with a correction for the truncated modes. The correction is facilitated by adding the energies of the truncated modes (given by their SPOD eigenvalues).

Figure 6 compares a single time instant of the original data in ($a$) with reconstructions of increasing fidelity in the frequency (left) and the time domain (right). Both the 1 $\times$ 129-mode reconstructions shown in figure 6($b$,$c$) capture the dominant wavepackets. However, the frequency-domain reconstruction lacks the detail of the time-domain reconstruction. The higher accuracy of the time-domain reconstruction can be explained by its less stringent nature. As the leading SPOD modes often represent a spatially highly confined structure, other structures associated with the same frequency cannot be represented by the frequency-domain reconstruction. The KH-type wavepacket seen in figure 3($c$) is a good example of such a confined structure. This difference between the approaches also explains the better reconstruction of the integral energy in the time domain, as previously observed in figure 4. The higher-dimensional versions for both approaches shown in figure 6($d$–$g$) yield increasingly more detailed and accurate reconstructions. Both approaches yield reconstructions that are indistinguishable from the original data when all modes are used (see figure 6$h$,$i$).

Figure 6.

Instantaneous pressure field: ($a$) original flow field is shown; ($b$,$d$,$\,f$,$h$) reconstructions in the frequency domain; ($c$,$e$,$g$,$i$) reconstructions in the time domain. Flow fields reconstructed using 1 $\times$ 129 modes, 3 $\times$ 129 modes, 10 $\times$ 129 modes and all modes are shown in ($b$,$c$), ($d$,$e$), ($\,f$,$g$) and ($h$,$i$), respectively. Contours in ($a$–$i$) are reported on the same colour axis.

We infer from figures 4–6 that reconstruction in the time domain provides a better estimate of the flow field than the frequency-domain version. To understand this observation, figure 7 reports the SPOD eigenspectra of the 1 $\times$ 129-mode reconstructions and compares them to those of the full data. Only the leading three eigenvalues are shown for clarity. The leading eigenvalue of the frequency-domain reconstruction in figure 7($a$) approximately follows the full data with some discrepancies at lower frequencies. No such discrepancies are observed for the time-domain reconstruction in figure 7($b$); in fact, the leading eigenvalue spectra are indistinguishable. Contrast this observation with the expectation that a $1\times n_{freq}$ frequency-domain reconstruction should exactly reproduce the leading-mode eigenspectrum, and that all higher-eigenvalue spectra are expected to be zero. In the context of figure 21 in Appendix A, we show that this is an effect of windowing that is not observed when using a rectangular window. The time-domain reconstruction, on the other hand, accurately approximates the first, and, to some degree, the leading suboptimal eigenvalue spectra. This again demonstrates the higher accuracy of the time-domain reconstruction that results from the higher flexibility of the expansion.

Figure 7.

Comparison between SPOD eigenvalue spectra of the original data (blue lines) and 1 $\times$ 129-mode reconstructions (red lines): ($a$) frequency domain; ($b$) time domain. Solid, dashed and dotted lines denote the first, second and third modes, respectively.

To quantify the accuracy of the two approaches, figure 8 compares their 2-norm errors as a function of the number of basis vectors (modes). For both the methods, the error reduces significantly as the number of modes retained per frequency increases from one to ten. For a fixed number of modes, the time-domain reconstruction is consistently more accurate. Recall that this is guaranteed by the optimality property of the oblique projection. It is, in fact, observed that the error of the time-domain reconstruction approaches machine precision for 40 or more modes per frequency. For the frequency-domain approach this only occurs for the full reconstruction using all modes.

Figure 8.

The 2-norm error of the pressure field reconstructed with different rank approximation: (red lines with squares) reconstruction in the frequency domain; (blue lines with circles) reconstruction in the time domain.

3.2. Denoising

After using SPOD truncation for the low-dimensional approximation previously described, we now explore its potential for denoising. We will show that additive noise is captured by certain parts of the spectrum, and that truncation of these parts leads to efficient denoising. This strategy is most efficiently implemented in the frequency domain. The local-in-time optimality of the time-domain approach is a hindrance in this context as it tends to reconstruct the noise. However, the one-to-one correspondence between modes and frequencies of the frequency-domain approach leads to efficient denoising.

We demonstrate denoising on additive Gaussian white noise, arguably the most common type of noise occurring in experimental environments. In particular, we add Gaussian white noise that has a standard deviation equal to the spatial mean of the standard deviation along the lipline of the pressure data. This scenario is very similar, for example, to heavily contaminated PIV data in which the variance of the noise is of the same order as the variance of the physical phenomena of interest. The SPOD eigenvalue spectrum of this noisy data is shown in figure 9($a$). Most noticeably, the addition of noise has introduced a noise floor at $\lambda \approx 4\times 10^{-5}$, effectively cutting off the spectrum at $\textit {St} \approx 1.5$. Information above this frequency lies below the noise floor and is not directly accessible. The leading eigenvalue of the original data (red dashed line) is shown for comparison. It lies well below the leading eigenvalue of the noisy data, which is elevated owing to the energy contained in the added noise. To illustrate the ability of SPOD to differentiate between spatially correlated, physical structures and noise, examples of modes that are above and below the noise floor are compared in figure 9($b$–$d$). The leading mode at $\textit {St}=0.5$ (figure 9$b$) clearly reveals the KH wavepacket and is indistinguishable from the corresponding mode of the original data shown in figure 3($a$). The fifth mode at $\textit {St}=0.5$ (figure 9$c$) and the leading mode at $\textit {St}=1.5$ (figure 9$d$), by contrast, are heavily contaminated by noise. The noise floor in the SPOD spectrum is found to be a very good indicator of this distinction. We therefore propose a denoising strategy based on hard thresholding of the spectrum. In this example, we pick a threshold of $5\times 10^{-5}$ (blue line), slightly above the noise floor. To address the effect of the truncation on the SPOD spectrum, we report the leading SPOD eigenvalue of the denoised data (magenta dashed line) in the same figure. It coincides with the leading eigenvalue of the noisy data up to the point where it intersects with the threshold limit, beyond which it falls off sharply, giving it the characteristics of a low-pass filter. A closer analysis of the truncated and original spectra reveals that the denoised field contains only $2.6\,\%$ of the energy of the noisy field, but that it contains $92.7\,\%$ of the energy of the original flow field. Another positive side effect is that only 74 out of 9933 modes ($n_{ freq} \times n_{ blk}$) have been retained, resulting in a space saving of $99.26\,\%$. These significant space savings are an advantage over standard denoising strategies based on low-pass filtering.

Figure 9.

The SPOD of data subjected to additive Gaussian white noise: ($a$) SPOD spectrum (black lines), leading SPOD eigenvalue of the original data (red dashed line), threshold of $5\times 10^{-5}$ (blue line) and the leading SPOD eigenvalue of the denoised data (magenta dashed line); ($b$) leading SPOD mode at $\textit {St}=0.5$; ($c$) fifth SPOD mode at $\textit {St}=0.5$; ($d$) leading SPOD mode at $\textit {St}=1.5$.

Representative instantaneous snapshots of the original data are compared with their noisy and denoised counterparts, and to the result of standard low-pass filtering in figure 10. The standard low-pass filter uses the cut-off frequency of $\textit {St}=0.8$ of the SPOD approach (inferred from figure 9) in the truncation of the long-time Fourier transform. A higher threshold, and its associated cut-off frequency, was found to lead to more aggressive filtering that can partially remove relevant flow structures. A threshold below the noise floor, on the other hand, leads to unsatisfactory noise rejection. In practice, a good trade-off between noise rejection and preservation of physically relevant flow structures is achieved by using the SPOD spectrum as a gauge to choose a threshold slightly above the noise floor. A comparison of the denoised data in figure 10($c$,$d$) with the noisy data in figure 10($b$) shows that significant noise reduction was achieved in all parts of the domain using both strategies. The resulting denoised flow fields clearly reveal the flow structures present in the original data. By visual inspection of the filtered pressure fields shown in figures 10($c$) and 10($d$), the SPOD-based strategy appears somewhat more efficient at removing the noise.

Figure 10.

Comparison of noisy and denoised instantaneous pressure fields: ($a$) original LES data; ($b$) LES data with additive Gaussian white noise; ($c$) SPOD-based denoised flow field; ($d$) low-pass filtered flow field. Denoising is achieved by rejecting all SPOD eigenpairs with $\lambda < 5\times 10^{-5}$. This hard threshold is indicated in figure 9.

For a more quantitative assessment, we compare the denoised flow fields in terms of two quantities. First, their signal-to-noise ratio (SNR) along the lipline, and second, the relative error between the denoised snapshots and the original data. The SNR is defined as

(3.2)\begin{equation} \textrm{SNR} = \frac{P_{ signal}}{P_{ noise}}= \frac{\sigma^{2}_{ signal}}{\sigma^{2}_{ noise}}, \end{equation}

where $P$ is power and $\sigma$ standard deviation. We further define the integral (over the physical domain) error as

(3.3)\begin{equation} \text{error} = \frac{\|\boldsymbol{q} - \boldsymbol{\check{q}}\|_x}{\|\boldsymbol{q}\|_x}, \end{equation}

where $\boldsymbol {q}$ and $\boldsymbol {\check {q}}$ are the original and the denoised flow fields, respectively. Figure 11($a$) compares the SNR along the lipline at $r=0.5$ for the noisy and the denoised flow fields. Both methods achieve an increase in the SNR over large parts of the domain. The low-pass filter performs better for $x\lesssim 10$, and the SPOD-based filter beyond that point. For $x\lesssim 2.5$, the SPOD-filtered pressure field exhibits a marginally lower SNR than the unfiltered data. We find that this is the result of the aggressive truncation of the high-frequency components by the SPOD-based filter. A result that is almost identical to that of the low-pass filter can be achieved by lowering the $\lambda$-threshold (a similar value for both methods is used here for consistency). Figure 11($b$) compares the time traces of the errors of the noisy and the two denoised flow fields. The error of the noisy data serves as a reference, and it is observed that both methods significantly reduce this error. The SPOD-based approach performs consistently better than the low-pass filter. This result is consistent with the visual observation of the denoised fields in figure 10($c$,$d$). Note that the threshold is an adjustable parameter in both methods. In practice, we find that by adjusting this parameter qualitatively very similar results can be obtained by both methods. This, however, leaves the SPOD-based approach with the advantage of significant data reduction.

Figure 11.

Comparison of the two denoising strategies: ($a$) the SNR along the lipline ($r=0.5$) for the noise added flow field (black line), SPOD-based denoised flow field (red lines), and the low-pass filtered flow field (blue line); ($b$) error of the noisy data, SPOD-based denoised data, and the low-pass filtered data. The amplitude of the additive noise was adjusted such that the average SNR along the lipline is one.

3.3. Frequency–time analysis

Intermittency, that is, the occurrence of flow events at irregular intervals, is an inherent feature of any turbulent flow. A common approach for the characterisation of intermittent behaviour is frequency–time analysis. Arguably the most commonly used tools of frequency–time analysis are WT and STFT. Their outcomes are scalograms and spectrograms, respectively, which indicate the presence of certain scales (WT), or frequency components (STFT), at certain times. Both methods are signal-processing techniques that are applied to one-dimensional time series, and therefore only quantify intermittency locally. As an alternative to this local perspective, we demonstrate how SPOD expansion coefficients can be used to study the intermittency of the spatially coherent flow structures represented by the modes. Next, frequency–time analyses based on both time-domain and frequency-domain reconstructions are introduced and compared.

3.3.1. Time-domain approach

We first consider the time-domain approach, in which the expansion coefficients obtained via oblique projection readily describe the temporal behaviour of each mode. The amplitudes of the expansion coefficients computed from (2.19), $|\sum _{j=1}^{n_{modes}}\tilde {a}^{(\,j)}(f_l,t)|$, hence, yield the desired frequency–time representation for the leading ${n_{modes}}$. The expansion coefficients are calculated using the full basis, i.e. $\tilde {\boldsymbol {{\phi }}}$ in (2.18), consists of all modes at all frequencies. Subsequently, we only consider the expansion coefficients of the leading $n_{{modes}}$ modes at each frequency. An alternative approach is to perform the oblique projection using a reduced basis that consists of only the leading $n_{{modes}}$ modes at each frequency. We find that the first approach is preferable in the context of frequency–time analysis and is explained in the Appendix B (see figure 22). The frequency–time diagrams for $n_{modes}=10$, and 1, are shown in figures 12($a$) and 12($b$), respectively. The leading 10 modes correspond approximately to $80\,\%$ of the total energy as shown in figure 2($b$). Most of the energy is concentrated at low frequencies, $St \lesssim 0.2$, as expected from the eigenvalue spectrum in figure 2. The eigenvalue spectrum provides a statistical representation of the structures that are coherent in space and time, whereas the frequency–time diagrams provide a temporal information of these structures. Bright yellow spots indicate high similarity of the instantaneous flow field with the leading mode in ($b$). These regions also correspond to high-energy events as we will show in figure 14.

Figure 12.

The SPOD-based frequency–time diagrams obtained using the time-domain approach: ($a$) first ten modes at each frequency; ($b$) leading mode at each frequency. The SPOD of the pressure field is considered.

3.3.2. Convolution-based approach

A direct way of using SPOD for frequency–time analyses is in terms of the SPOD expansion coefficients. Since each block is associated with a finite time interval, this approach requires the computation of SPOD using an overlap of $n_{ ovlp}= n_{ fft} - 1$ to obtain time-resolved coefficients (Towne & Liu Reference Towne and Liu2019). This approach assumes that the value of the expansion coefficient obtained from a finite time segment (block) represents the instantaneous frequency content at the centre of the time segment. A limitation of this approach is its high memory requirement (3.6 TB for the present example). As an alternative, we propose a computationally tractable way of calculating time-continuous expansion coefficients based on the convolution theorem. Applying the convolution theorem to the inverse SPOD problem yields

(3.4)\begin{align} \boldsymbol{a}_l^{(i)}(t) &= \left(\boldsymbol{\phi}_l^{(i)} \exp({-\textrm{i} 2{\rm \pi} f_l t}) \circledast \boldsymbol{q}\right) (t)\nonumber\\ &=\int_{\Delta T} \int_{\varOmega} \left( \boldsymbol{\phi}_l^{(i)}(x)\right)^{*}\boldsymbol{W}(x)\boldsymbol{q}(x,t+\tau)w(\tau) \exp({-\textrm{i} 2{\rm \pi} f_l\tau})\,\mathrm{d}\kern0.7pt x\, \mathrm{d} \tau, \end{align}

where $\circledast$ indicates the convolution between the time evolving SPOD mode and the data, which takes into the account the windowing function, $w(\tau )$, and the weight matrix, $\boldsymbol{W}$. In practice this convolution is computed by expanding the SPOD mode in time as $\boldsymbol {\phi }_l^{(i)} \exp ({-\textrm {i} 2{\rm \pi} f_l t})$ and convolving it over the data one snapshot at a time. In this step, we leverage the orthogonality property of the SPOD mode in the space–time inner product, which allows us to compute the expansion coefficient one at a time. If the SPOD was computed using an overlap of $n_{ fft}$-1, then the expansion coefficients, $\boldsymbol {a}_l^{(i)}$, obtained from (3.4) and (2.13) are mathematically identical. Here, the underlying idea is to apply the continuously discrete convolution integral to the SPOD mode computed with a significantly lower overlap to make it computationally feasible. We confirmed that the frequency–time diagrams of the expansion coefficients obtained using (3.4) for an overlap of $50\,\%$ are virtually indistinguishable to those obtained from (2.13) for an $n_{{ovlp}} = n_{fft}-1$ (shown in the Appendix C, figure 24). This is to be expected since the convergence of the SPOD modes does not improve significantly for overlap over $50\,\%$. In practice, the convolution integral in (3.4) is most efficiently computed using fast-Fourier transforms.

Frequency–time diagrams of the expansion coefficients for the convolution approach are shown in figure 13. Figure 13($a$) and 13($b$) show the contribution of the leading ten modes and the leading mode, respectively. These frequency–time diagrams appear less detailed compared to the frequency–time diagrams of the time-domain approach. In the context of figure 15, though, we will show that figures 12 and 13 basically contain the same information. For now, it is sufficient to note that the convolution and time-domain approaches detect the same trends. Take as an example, the high energy events occurring at low frequency in the time ranges, $550 \lesssim t \lesssim 590$ and $1370 \lesssim t \lesssim 1400$, in the spectrograms of figures 12($b$) and 13($b$).

Figure 13.

The SPOD-based frequency–time diagrams obtained using the convolution approach: ($a$) first ten modes at each frequency; ($b$) leading mode at each frequency. The SPOD of the pressure field is considered. The cyan box in ($b$) is centred around the global maximum of the instantaneous energy at $t=1380$, analysed in figures 14 and 15($c$,$d$) below.

Figure 14.

Temporal evolution of the pressure 2-norm in the vicinity of its global maximum at $t=1380$. The convolution approach, based on (3.4), is compared to the time- and frequency-domain approaches, previously shown in figure 4($b$,$d$). The 1 $\times$ 129-mode reconstructions are shown.

Figure 15.

Oblique projection and convolution-based expansion coefficients of the leading mode at $\textit {St}=0.5$ (top) and $\textit {St}=0.05$ (bottom): ($a$,$c$) time traces in the vicinity of their global maximum (black dashed line); ($b$,$d$) cross-correlation of the expansion coefficients obtained using the two different approaches. The black dash-dotted line denotes the weighted moving mean of the time-domain expansion coefficient. The moving mean uses as weights the same Hamming windowing function as the SPOD.

3.3.3. Comparison of methods and interpretation of results

Next, we investigate if the high similarity between the instantaneous flow field and the modes indicates high energy. Figure 14 shows the temporal evolution of the pressure 2-norm for the original data, low-dimensional 1 $\times$ 129-mode reconstructions using the time-domain, frequency-domain and the convolution approaches. The pressure 2-norm of the data is highly underpredicted by the time-domain approach that uses a full basis ($n_{ blk}\times$129), but is able to capture the major trends of the original data. The time-domain reconstruction performed using a modal basis of 1 $\times$ 129 is also shown for comparison. This accurately follows the spatial norm of the original data, except for an offset, similar to figure 4($d$). The frequency-domain curve also shows a similar trend. In addition, the spatial norm of the 1 $\times$ 129-mode reconstruction using the convolution approach is shown. It follows the trend of the original data and attains its global maximum at the same time instant. Minor differences between the convolution (time-continuous) and frequency-domain (50 % overlap) approaches are expected, see Appendix C. All curves in figure 14 peak at the time of maximum instantaneous energy, previously indicated in figure 13($b$). This indicates that a high similarity between the instantaneous flow field and the leading mode implies high overall energy. We highlight that this finding is not self-evident as the leading SPOD mode represents the most energetic flow structure in a purely statistical sense. The important physical insight is that the intermittent occurrence of large-scale coherent structures is directly associated with high-energy events.

To understand the qualitative differences of the frequency–time diagrams in figures 12 and 13, we now look at the expansion coefficients of the two approaches. Figure 15 compares the expansion coefficient of the leading mode, obtained by the time-domain and convolution approaches. As an example, the expansion coefficient at $St \approx 0.50$ is shown in figure 15($a$). It is centred around its global maximum, in the time interval $1000 \le t \le 1300$. We observe that the time traces of the expansion coefficients obtained from the two approaches show similar trends. In particular, the local peaks occur at similar locations, with both curves exhibiting the global maximum at $t=1150$ (black dashed line). Compared to the time-domain approach, the convolution curve is smoother and resembles a moving average of the time-domain curve (black dash-dotted line). For optimal comparison with the convolution approach, the moving average is computed by weighting the time-domain curve by the Hamming window in (2.6) and averaging over 256 points. To further quantify the relation between the expansion coefficients of the two approaches, we show the cross-correlation coefficient in figure 15($b$). The cross-correlation coefficient confirms the observation that the expansion coefficients obtained from the two approaches are similar, by demonstrating a cross-correlation coefficient of 0.77 at $0$-time lag ($\tau = 0$). We have confirmed that this correspondence holds in general. In figures 15($c$) and 15($d$), for example, the same trends are observed for the expansion coefficients at the lower frequency of $\textit {St}=0.05$ over the time interval previously shown in figure 14. From figure 15, we infer that the intermittency of the coherent structures can be captured using both approaches.

After establishing the correspondence between the time-domain and convolution approaches, we now compare the spectral characteristics of the two approaches. The PSD of the expansion coefficients associated with the leading mode at $\textit {St}=0.2$, 0.5 and 1.0, for the time and convolution-domain approaches are shown in figure 16($a$). As expected the PSD peak at the frequency of the corresponding mode for both approaches. The expansion coefficients computed in the convolution approach exhibit a much narrower peak than those in the time-domain approach. Note that, we cannot expect a sharp spectral peak even for the convolution approach owing to spectral leakage and the modulation of the wave amplitude as seen in figure 15. Figure 16($c$) compares the PSD of the leading mode and the ten leading modes at $\textit {St} = 0.5$, which underlines the dominance of the leading mode at this particular frequency. The expansion coefficients are presented in terms of the spectral energy content in figure 16($b$,$d$). As the expansion coefficients are uncorrelated, and their expected value is equal to the SPOD modal energy,

(3.5)\begin{equation} E{\left\{{\boldsymbol{a}_f^{(i)}\boldsymbol{a}_f^{(\,j)}}\right\}}=\lambda_f^{(i)} \delta_{ij}, \end{equation}

it is expected that the convolution approach accurately approximates the eigenvalue spectrum. The blue and magenta lines are almost coincident in figure 16($b$,$d$), thus confirming this conjecture. For the time-domain approach, the expected value for the sum of first 10 modes approximates the total integral PSD for all but the low frequencies $\textit {St} \ge 0.2$ in figure 16($d$). On considering only the first eigenvalue, the time-domain approach underpredicts the eigenvalue spectrum for $\textit {St} \le 1.0$, (figure 16$b$). Note that, this observation does not contradict the observations made in context of figure 4, as the expansion coefficients are obtained from a full basis here, but from a smaller basis in figure 4($d$).

Figure 16.

Spectral analysis of the expansion coefficients for the time-domain and convolution approaches: ($a$) PSD of the individual expansion coefficients of the leading SPOD mode at $\textit {St} = 0.2$, $0.5$ and $1.0$; ($b$) expected values of the expansion coefficients of the leading mode; ($c$) PSD of the expansion coefficients of the leading mode and sum of the first ten leading modes (line with squares) at $\textit {St} = 0.5$; and ($d$) expected value of the expansion coefficients for the sum of the first ten modes. In ($b$,$d$), the leading, sum of leading 10, and sum of all eigenvalues are shown for comparison.

After examining the properties of the expansion coefficients, we focus on the spatial composition of the reconstructed flow field in terms of contributions from individual modes in figure 17. The time instant of high energy, previously marked in figure 15, is chosen as an example. The contribution of the leading SPOD modes at two representative frequencies, $\textit {St}=0.5$, and 0.05, to the original flow field is shown in figure 17. Figure 17($b$,$c$) show the modes weighted by their expansion coefficient, $a^{(1)}\phi ^{(1)}$ at the corresponding time instant of these two frequencies. Close to the nozzle exit, the LES flow field clearly exhibits a KH-type instability wave. The leading mode at $\textit {St}=0.5$ closely resembles this structure. Similarly, the dominant wave pattern with a large wavelength ($\approx 5$) observed in the flow field is represented by the mode at $\textit {St}=0.05$ in a location downstream of the potential core ($12\lesssim x\lesssim 20$). The real part of the pressure field along the lipline ($r=0.5$) is compared with the contributions of the leading modes at $\textit {St}=0.5$ and $\textit {St}=0.05$ in figures 17($d$) and 17($e$), respectively. It can be seen that the phases of the pressure field and the mode at $\textit {St}=0.5$ are aligned in the region where the mode attains its maximum. A weaker but similar kind of phase alignment is also observed for low frequency, $\textit {St}=0.05$, despite the disturbed nature of the wavepacket in the region, $12\lesssim x \lesssim 20$. For the flow field at the current time instant, this also explains that the contribution of the leading mode at $\textit {St}=0.05$ is lower than $\textit {St}=0.5$, where the KH wavepacket dominates the flow field. These observations confirm that the maximum in the frequency–time diagrams indicate close resemblance of the instantaneous flow field with the corresponding SPOD modes. Since the SPOD modes are the most energetic structures it is not surprising that the maxima in the frequency–time diagrams indicate the intervals of high energy. Furthermore, as the leading SPOD modes are spatially coherent and contain the most energy at each frequency, we infer that SPOD-based frequency–time analysis can be used to gauge the intermittency of large-scale coherent structures. Here, for brevity, only the convolution approach is shown, but we note that these conclusions also hold for the time-domain approach.

Figure 17.

Contributions of individual modes to the reconstructed flow field: ($a$) instantaneous pressure field; ($b$) contribution of ${\phi }^{(1)}$ for $St=0.5$ and ($c$) for $St=0.05$; ($d$) and ($e$) comparisons of the real part of the pressure field along the lipline ($r=0.5$) for $St=0.5$ and $St=0.05$, respectively. The instantaneous flow field at $t=1150$ (see figure 15) is shown. Contours in ($a$–$c$) are reported on the same colour axis.

3.4. Prewhitening

As mentioned in § 1, prewhitening is a filtering operation that results in a flat power spectrum, and is commonly used for trend detection in atmospheric and geophysical applications. The goal, therefore, is to use SPOD to scale the data in order to have the same energy at all frequencies. We propose to achieve this goal by rescaling the expansion coefficients of the reconstruction in the frequency domain. The frequency-domain approach is chosen for the same reasons as for denoising in § 3.2. We leverage the fact that the expansion coefficients are uncorrelated, and that their expected value is equal to SPOD modal energy

(3.6)\begin{equation} E{\left\{{\boldsymbol{a}_f^{(i)}\boldsymbol{a}_f^{(\,j)}}\right\}}=\lambda_f^{(i)} \delta_{ij}. \end{equation}

We propose two different scalings,

(3.7)\begin{gather} \frac{\sqrt{\sum_f \sum_i \lambda_f^{(i)}}}{\sqrt{\lambda_f^{(i)}}}\boldsymbol{a}_f^{(i)} \quad(\text{scaling}\ 1) \end{gather}

and

(3.8)\begin{gather}\frac{1}{\sqrt{\sum_i\lambda_f^{(i)}}}\boldsymbol{a}_f^{(i)} \quad(\text{scaling}\ 2) \end{gather}

to scale the integral mode energy, that is, the sum of all eigenvalues, to one at each frequency. Both methods achieve this goal, but result in different relative scalings of individual SPOD modes. Figures 18($a$) and 18($b$) show the effect of the two scalings on the SPOD eigenvalue spectrum. The reconstructed flow fields obtained from the expansion coefficients scaled using (3.7) and (3.8) are shown in figures 18($c$) and 18($d$), respectively. Note that (3.7) collapses all eigenvalues in figure 18($a$) to the same value. Scaling 2, on the contrary, preserves both the mode hierarchy and the relative energy content. In comparison to the original flow field shown in figure 6($a$), prewhitening emphasises high-frequency structures in the shear layer, whereas it de-emphasises the highly energetic large-scale structures associated with low frequencies downstream of the potential core. This portrayal of the flow field might appear unfamiliar; we emphasise that the objective of prewhitening is not physical interpretation, but pattern identification. Here, for example, the prewhitened pressure fields bring to light the trapped acoustic modes in the potential core. These modes have only recently been described in detail (Schmidt et al. Reference Schmidt, Towne, Colonius, Cavalieri, Jordan and Brès2017b; Towne et al. Reference Towne, Cavalieri, Jordan, Colonius, Schmidt, Jaunet and Brès2017). Previously, they remained largely unnoticed in the analysis of jet data because of their low energy content. An important difference between SPOD-based prewhitening and classical local, point-wise prewhitening techniques is that the SPOD-based approach preserves the spatial coherence of the flow structures identified by the SPOD modes.

Figure 18.

The SPOD-based prewhitening: ($a$,$b$) rescaled SPOD spectra; ($c$,$d$), instantaneous pressure fields using definitions (3.7) and (3.8), respectively. Red lines indicate the sum of all eigenvalues, that is, the integrated PSD. All lines in ($a$) collapse owing to the scaling. The original SPOD eigenvalue spectrum can be seen in figure 2($a$).