2.1 Numerical method and flow initialisation

We solve (1.1) using contour advection performed by the combined Lagrangian advection method (Dritschel & Fontane Reference Dritschel and Fontane2010) on a $1024^{2}$ basic inversion grid with effective resolution $(16\cdot 1024)^{2}=16\,384^{2}$ and 80 contour levels used to represent PV. The domain side length is $2\unicode[STIX]{x03C0}$ and the deformation wavenumber is set to $\unicode[STIX]{x1D706}=40$ , corresponding to $L_{D}=1/40$ , or $65/16\,384$ th the domain width. Contour surgery removes PV filaments at $1/16\,384$ th the domain width, but preserves sharp gradients indefinitely, so is ideally suited to investigating dynamics associated with PV fronts.

We initialise the simulation with the spatially random smooth PV field pictured in figure 1(a). Concentrations of PV are present in this initial field: positive maxima are red and negative minima are blue. These concentrations merge and evolve into small vortices, much as coherent vortices evolve from extrema of the initial vorticity field in freely evolving barotropic turbulence (see Burgess, Dritschel & Scott Reference Burgess, Dritschel and Scott2017, and references therein).

Figure 1.

(a) Initial PV field and (b) spectrum ${\mathcal{C}}(k)$ as defined in (2.1).

We denote the power spectrum of $C\equiv \langle q^{2}\rangle /2$ as ${\mathcal{C}}(k)$ . The initial spectrum, shown in figure 1(b), takes the form

(2.1) $$\begin{eqnarray}{\mathcal{C}}(k)=c(k_{d}^{2}+k^{2})k^{2p-3}\text{e}^{-(p-1)(k/k_{0})^{2}},\end{eqnarray}$$

where we choose $p=3$ and $k_{0}=40$ , so that the initial spectrum is peaked at $k_{0}=\unicode[STIX]{x1D706}$ , and the characteristic length scale of the initial PV field is the deformation length $L_{D}=1/40$ . The constant $c$ is chosen so that $|q|_{max}=4\unicode[STIX]{x03C0}$ , giving a unit rotation period for a circular vortex of size $L\ll L_{D}$ . Note that while this is the relevant time scale for vortices much smaller than  $L_{D}$ , it is not the relevant time scale for flow features much larger than  $L_{D}$ , such as the large mixed PV patches and bounding jets we study below. The simulation was carried out until $t=640\,000$ , though PV gradient sharpening and the emergence of fronts occurs relatively early, by $t\sim 10\,000$ .

2.2 Flow regime

Figure 2 shows how the quadratic invariants energy $E=K+P$ and potential enstrophy $Q=Z+\unicode[STIX]{x1D706}^{2}K$ are each partitioned between their two terms. In panel (a) are plotted the potential enstrophy $Q$ (dash-dot line), which decays in time, and the energy $E$ (solid line), which is conserved. As shown in panel (b), at $t=100$ , $K/P\approx 0.3$ and decreases steadily thereafter (solid line), while $P/E$ approaches 1 at late times (dash-dot line), showing the dominance of the potential energy in the flow. Panel (c) shows that the rescaled kinetic energy $\unicode[STIX]{x1D706}^{2}K$ makes the dominant contribution to the potential enstrophy, with $\unicode[STIX]{x1D706}^{2}K/Q\approx 0.75$ at late times (dash-dot line). The ratio between the two terms $Z$ and $\unicode[STIX]{x1D706}^{2}K$ in the potential enstrophy $Q$ show no systematic growth or decay, with $Z/\unicode[STIX]{x1D706}^{2}K\approx 0.3$ at late times (solid line) – this is because the two terms decay roughly the same way, as will be discussed below.

Figure 2.

(a) Potential enstrophy $Q$ and energy $E$ as functions of  $t$ , (b) ratios $P/E$ of potential to total energy and $K/P$ of kinetic to potential energy, and (c) ratios $\unicode[STIX]{x1D706}^{2}K/Q$ of rescaled kinetic energy to potential enstrophy and $Z/\unicode[STIX]{x1D706}^{2}K$ of enstrophy to rescaled kinetic energy.

The spectra of total, kinetic, and potential energy are, respectively,

(2.2a-c ) $$\begin{eqnarray}{\mathcal{E}}(k)=\frac{{\mathcal{C}}(k)}{k^{2}+\unicode[STIX]{x1D706}^{2}},\quad {\mathcal{K}}(k)=\frac{k^{2}{\mathcal{C}}(k)}{(k^{2}+\unicode[STIX]{x1D706}^{2})^{2}},\quad {\mathcal{P}}(k)=\frac{\unicode[STIX]{x1D706}^{2}{\mathcal{C}}(k)}{(k^{2}+\unicode[STIX]{x1D706}^{2})^{2}},\end{eqnarray}$$

and are shown in figure 3 at (a)  $t=10\,000$ and (b)  $t=400\,000$ . For $k>\unicode[STIX]{x1D706}$ , ${\mathcal{E}}(k)\approx {\mathcal{K}}(k)$ , while for $k<\unicode[STIX]{x1D706}$ , ${\mathcal{E}}(k)\approx {\mathcal{P}}(k)$ . The large-scale flow is thus strongly dominated by potential energy. As can be seen by comparing panels (a) and (b), the peak of the potential energy spectrum moves to larger scales as time proceeds, indicating an inverse cascade of potential energy. Meanwhile the kinetic energy is depleted at scales $L>L_{D}$ , evident from comparing $\log _{10}[{\mathcal{K}}(k)]$ (red dash-dot curve) at large scales in panels (a) and (b). Hence, though the flow is in the potential energy regime it remains dynamically active, with an ongoing inverse cascade of potential energy and dissipation of kinetic energy.

Figure 3.

Spectra ${\mathcal{E}}(k)$ , ${\mathcal{K}}(k)$ , and ${\mathcal{P}}(k)$ at (a)  $t=10\,000$ and (b)  $t=400\,000$ .

3.1 Emergence of PV jumps and mixed regions

As early as $t=10\,000$ the PV field begins to develop sharp jumps, which emerge along with regions in which PV is nearly homogenised, while the length scale of the flow increases. Figure 4 shows the PV field at three times in panels (a–c), with the corresponding kinetic energy fields directly below in panels (d–f). The times are equally spaced in $t^{1/3}$ for reasons that will become clear below. As is evident, the spatially random initial PV field evolves into a collection of vortices, the largest having a wedding cake structure, with layers formed by plateaus of mixed PV whose value increases in a step-like fashion towards the central core. This structure is consistent with that observed in previous simulations of freely evolving equivalent barotropic flow (Arbic & Flierl Reference Arbic and Flierl2003). The well-mixed regions are visible in figure 4(a–c) as green and yellow (positive) and light-dark blue (negative) patches around the more intense vortex cores. The sharp PV jumps bounding the plateaus of the staircase vortices are collocated with strong jets, visible as cyan and dark blue ‘ropes’ in figure 4(d–f), which become more well defined as time proceeds.

Figure 4.

(a–c) PV fields and (d–f) corresponding kinetic energy density fields. (a) PV field at $t=27\,000$ , (b) PV field at $t=125\,000$ , (c) PV field at $t=343\,000$ , (d) KE field at $t=27\,000$ , (e) KE field at $t=125\,000$ , (f) KE field at $t=343\,000$ .

The movies in the supplementary materials, available at https://doi.org/10.1017/jfm.2019.133, show the flow in motion: Movie 1 shows the kinetic energy field, while Movie 2 shows the PV field over the same range of times. The flow actually consists of two subpopulations of vortices, which are dynamically distinct: there are large active vortices with wavy boundaries, which drift slowly, interacting with each other and occasionally colliding. During these collisions their surrounding jets split and reconnect, ejecting tendrils of kinetic energy and forming disturbances with radius of curvature $O(L_{D})$ , which then propagate along the jets, continuing to shed kinetic energy as they smooth out and the jets regain their integrity. There are also relatively small, circular vortices whose boundaries do not support waves, and which display AM-regime-type behaviour, sitting in one location for extended periods of time, until a large active vortex sweeps them up or propels them into another vortex. These small dynamically inactive vortices resemble a remnant of the vortical quasi-crystal observed in prior studies.

Figure 5 shows the development of the staircase structure. We plot the total area $A(q\geqslant q_{thr})$ of the regions on which the PV exceeds a threshold $q_{thr}$ at times $t=1000$ , 27 000, 125 000, and 664 000. The value of $q_{thr}$ is not fixed, but rather is varied as indicated on the horizontal axis to generate the staircase plot. By $t=27\,000$ (dotted blue line) a clear staircase structure has already developed, indicating the emergence of sharp fronts. There are two primary non-zero values of mixed PV for both $q<0$ and $q>0$ . A similar plot for the streamfunction (not shown) has the same primary steps, reflecting the dominance of the streamfunction in the large-scale PV distribution. The PV staircase is sharper than the $\unicode[STIX]{x1D713}$ staircase due to small-scale structure (the non-negligible vorticity field in the shear layers on the jet flanks) in the vicinity of the fronts and the effect of PV inversion in $\unicode[STIX]{x1D713}=(\unicode[STIX]{x0394}-\unicode[STIX]{x1D706}^{2})^{-1}q$ .

Figure 5.

Area $A(q\geqslant q_{thr})$ on which $q\geqslant q_{thr}$ .

In the absence of contour surgery the $A(q\geqslant q_{thr})$ curve would be invariant: the emergence of the staircase depends crucially on filament shedding and coarse-graining of PV through surgery. We note that if a small viscous term were used instead of contour surgery, dissipation would occur evenly along the fronts. In contrast, surgery only occurs when there are events such as reconnections that disrupt the integrity of the jets and generate small-scale features that actually lead to filament shedding. These disruptive events and the resulting small-scale structures should be distinguished from the $O(L_{D})$ cross-section of the front itself, which is a long-lived coherent structure resistant to filamentation. In other words, contour surgery dissipates the correct small-scale structures, allowing us to represent destructive events while simulating the inviscid dynamics of the fronts as faithfully as possible.

In figure 6, we plot the total circulation of regions with a given value of PV. In this plot the PV intervals reflect the contour levels used, and the well-mixed regions show up as large spikes at $q\approx \pm 3$ and $q\approx \pm 5.5$ . These spikes grow in time, while the area at adjacent values of $q$ is depleted, reflecting the net growth of mixed regions through entrainment and mixing of surrounding PV. The spikes at $q\approx \pm 3$ are the largest, so these values of mixed PV, which lie in the lowest levels of the staircase vortices, i.e. the green and light blue regions in figure 4(a–c), are associated with the largest total circulation. The tertiary spikes at $q\approx \pm 5.5$ correspond to the second mixed levels within the vortices, i.e. the dark blue and yellow regions in figure 4(a–c).

Figure 6.

Total circulation $\unicode[STIX]{x1D6E4}(q)$ of regions on which PV takes the value  $q$ . Times $t=10\,000$ , $t=200\,000$ and $t=600\,000$ are indicated for reference.

3.2 Scaling theory

PV gradient sharpening, mixing, and vortex merger occur through the interaction of the wavy, undulating vortex boundaries. These interlinked dynamical processes drive the growth of the flow’s characteristic length scale and the decay of quantities supported on and in the vicinity of the PV fronts, which occurs when frontal length is lost as a result of vortex mergers. Potential enstrophy  $Q$ , rescaled kinetic energy $\unicode[STIX]{x1D706}^{2}K$ , and enstrophy $Z$ are plotted as functions of time in figure 7(a). Both $\unicode[STIX]{x1D706}^{2}K$ and $Q$ decay as $t^{-1/3}$ , as does  $Z$ , though more roughly and at comparatively later times.

Figure 7.

(a) Decays of the potential enstrophy  $Q$ , rescaled kinetic energy $\unicode[STIX]{x1D706}^{2}K$ , and enstrophy  $Z$ , with a $t^{-1/3}$ line for comparison, and (b) growth in time of the non-dimensionalised typical vortex radius $R_{typ}/L_{D}$ , average vortex radius $R_{av}/L_{D}$ with best-fit line  $t^{0.32}$ , and characteristic area $(l_{s}/L_{D})^{2}$ with best-fit line  $t^{0.34}$ .

We now show that the decay rates of these quantities can be deduced using a scaling argument. We consider $N$ vortices with characteristic radius $R$ supporting long frontal waves of wavelength $\unicode[STIX]{x1D6EC}$ on their boundaries. We identify the frequency $\unicode[STIX]{x1D714}$ of the long waves with an inverse time, $\unicode[STIX]{x1D714}\sim 1/t$ . In essence we are assuming that the long-wave period is the relevant time scale for the large-scale dynamics. We also require $\unicode[STIX]{x1D6EC}\sim R$ , which amounts to assuming self-similar growth in time: if the vortex radius $R$ is rescaled by some factor, then so is the wavelength $\unicode[STIX]{x1D6EC}$ of the long waves. This assumption is also consistent with previous work, which has found that both steady and unsteady evolving vortex patches exhibit boundary waves with length scales comparable to the vortex perimeter, and therefore $R$ (Płotka & Dritschel Reference Płotka and Dritschel2012). Using the relationship $\unicode[STIX]{x1D714}\sim (L_{D}/\unicode[STIX]{x1D6EC})^{3}$ for long waves in the thin-jet limit (Nycander et al. Reference Nycander, Dritschel and Sutyrin1993) together with $\unicode[STIX]{x1D6EC}\sim R$ then yields

(3.1) $$\begin{eqnarray}R\sim t^{1/3}.\end{eqnarray}$$

Since PV is materially conserved, we expect the total area enclosed within the vortices to be constant, $NA\sim NR^{2}=\text{const.}$ ; this implies

(3.2) $$\begin{eqnarray}N\sim R^{-2}\sim t^{-2/3}.\end{eqnarray}$$

Finally, the total perimeter of the vortices scales as $L_{F}\sim NR$ , so

(3.3) $$\begin{eqnarray}L_{F}\sim t^{-1/3}.\end{eqnarray}$$

Kinetic energy $K$ is concentrated in the jets, while potential enstrophy $Q$ and enstrophy $Z$ are concentrated in shear layers of width $O(L_{D})$ on the jet flanks, so it follows that

(3.4a-c ) $$\begin{eqnarray}K\sim t^{-1/3},\quad Q\sim t^{-1/3},\quad Z\sim t^{-1/3}.\end{eqnarray}$$

These are indeed the decay laws observed in figure 7(a).

The scaling theory also predicts in (3.1) above that the typical staircase vortex radius $R$ grows like $R\sim t^{1/3}$ and that the number of vortices decays like $N(t)\sim t^{-2/3}$ . To check these predictions we first identify vortices using a threshold of $q_{rms}$ on PV, which due to the staircase structure extracts vortices cleanly and with no ambiguity. As discussed above in § 3.1, the flow consists of two subpopulations of vortices: large drifting vortices with wavy boundaries, and small circular vortices that remain almost stationary for long periods of time and whose boundaries do not support waves. Since our theoretical considerations above apply to the active vortices with wavy boundaries, we must exclude the relatively inactive circular vortices from the average. It is easy to exclude the relatively inactive circular vortices because they are comparatively small, not having undergone as many mergers as the large vortices. Note that using a cutoff of $O(L_{D})$ would contaminate the scaling behaviour with $O(L_{D})$ effects. One would only expect structures sufficiently large compared to the characteristic scale $L_{D}$ to exhibit self-similarity. We thus impose a lower bound of half a typical vortex area $A_{typ}$ on vortices included in the average, where $A_{typ}$ is defined as

(3.5) $$\begin{eqnarray}A_{typ}\equiv \frac{\displaystyle \mathop{\sum }_{i=1}^{N_{\text{tot}}(t)}A_{i}^{2}q_{i}^{2}}{\displaystyle \mathop{\sum }_{i=1}^{N_{\text{tot}}(t)}A_{i}q_{i}^{2}}.\end{eqnarray}$$

Here $A_{i}$ is the area of vortex $i$ , $q_{i}$ is the PV averaged over vortex $i$ and $N_{\text{tot}}(t)$ is the total number of vortices, with small vortices included in this initial sum. The choice of this definition for $A_{typ}$ is motivated by the findings of Burgess et al. (Reference Burgess, Dritschel and Scott2017). We also tried a lower bound of half the average vortex area (where the initial average includes the small vortices): both choices of lower bound yield equivalent results. The average vortex area $A_{av}$ is then defined as the sum of all vortex areas having $A_{i}>A_{typ}$ divided by the number of such vortices.

Figure 7(b) shows $R_{typ}/L_{D}$ , where $R_{typ}=\sqrt{A_{typ}}$ , and $R_{av}/L_{D}$ , which grows like $t^{0.32}$ (dotted magenta least squares best-fit line), very close to the predicted $t^{1/3}$ . Moreover $R_{typ}$ almost coincides with $R_{av}$ . The difference is greatest at earlier times, and decreases as the active vortices with undulating boundaries grow ever larger and increasingly dominate both quantities. Also shown is $(\ell _{s}/L_{D})^{2}$ , where

(3.6) $$\begin{eqnarray}\ell _{s}=\sqrt{E/Q}\end{eqnarray}$$

is a characteristic length scale that was identified with the potential enstrophy centroid by Tran & Dritschel (Reference Tran and Dritschel2006), who assumed it to be conserved for flows with smooth PV fields. Figure 7(b) shows that when sharp gradients and small length scales are present in the PV field, $\ell _{s}$ is not conserved; rather $(\ell _{s}/L_{D})^{2}\sim t^{0.34}$ as indicated by the dotted cyan least squares best-fit line.

Figure 8 shows the number of vortices $N(t)$ (solid black line) with areas exceeding the cutoff area $A_{typ}/2$ as a function of time. At late times the curve becomes noisy because the flow is dominated by a few large vortices. As shown by the least squares best-fit line (dotted magenta) the number of vortices $N(t)$ decays as $t^{-0.64}$ , close to the predicted  $t^{-2/3}$ .

Figure 8.

Number of vortices $N(t)$ exceeding the cutoff $A_{typ}/2$ as a function of time, with best-fit line  $t^{-0.64}$ .

To gain more physical insight into the area $\ell _{s}^{2}$ , we rewrite $\ell _{s}$ as

(3.7) $$\begin{eqnarray}\ell _{s}=\sqrt{\frac{\langle -\unicode[STIX]{x1D713}q\rangle }{\langle \unicode[STIX]{x0394}\unicode[STIX]{x1D713}q\rangle }}=\sqrt{\frac{\langle |\unicode[STIX]{x1D735}\unicode[STIX]{x1D713}|^{2}\rangle +\unicode[STIX]{x1D706}^{2}\langle \unicode[STIX]{x1D713}^{2}\rangle }{\langle |\unicode[STIX]{x0394}\unicode[STIX]{x1D713}|^{2}\rangle +\unicode[STIX]{x1D706}^{2}\langle |\unicode[STIX]{x1D735}\unicode[STIX]{x1D713}|^{2}\rangle }}\end{eqnarray}$$

and then make approximations appropriate to the potential-energy-dominated regime, neglecting kinetic energy in the numerator and enstrophy in the denominator, such that

(3.8) $$\begin{eqnarray}\ell _{s}\approx \sqrt{\frac{\langle \unicode[STIX]{x1D713}^{2}\rangle }{\langle |\unicode[STIX]{x1D735}\unicode[STIX]{x1D713}|^{2}\rangle }}.\end{eqnarray}$$

We again consider $N$ vortex patches with typical radius $R$ and values of mixed PV $q\approx \pm \unicode[STIX]{x1D706}^{2}\unicode[STIX]{x1D6F9}_{0}$ , where the vortices can be positive or negative and $\unicode[STIX]{x1D6F9}_{0}$ is the typical magnitude of the streamfunction on the patches. (Note that inside the vortices away from the boundaries, PV is dominated by the streamfunction, $q\approx -\unicode[STIX]{x1D706}^{2}\unicode[STIX]{x1D713}$ ). This is actually a very good approximation, as can be seen by examining figure 6, which shows that most of the flow’s circulation is concentrated at $q\approx \pm 3$ . The support of the potential energy is then proportional to $NR^{2}$ , while that of the kinetic energy, which is concentrated in jets of width $L_{D}$ and typical length $R$ on the boundaries, is proportional to $NRL_{D}$ . Hence

(3.9) $$\begin{eqnarray}\ell _{s}^{2}\approx \frac{\langle \unicode[STIX]{x1D713}^{2}\rangle }{\langle |\unicode[STIX]{x1D735}\unicode[STIX]{x1D713}|^{2}\rangle }\sim \frac{NR^{2}\cdot \unicode[STIX]{x1D6F9}_{0}^{2}}{NRL_{D}\cdot L_{D}^{-2}\unicode[STIX]{x1D6F9}_{0}^{2}}=RL_{D}.\end{eqnarray}$$

This shows that $\ell _{s}^{2}$ is proportional to the area $RL_{D}$ to be consistent with equation (3.9) occupied by a typical PV front.