Prospects of Turbulence Studies in HighEnergy Density LaserGenerated Plasma:
Numerical Investigations in Two Dimensions
Abstract
We investigate the possibility of generating and studying turbulence in plasma by means of highenergy density laserdriven experiments. Our focus is to create supersonic, selfmagnetized turbulence with characteristics that resemble those found in the interstellar medium (ISM).
We consider a target made of a spherical core surrounded by a shell made of denser material. The shell is irradiated by a sequence of laser pulses sending inwardpropagating shocks that convert the inner core into plasma and create turbulence. In the context of the evolution of the ISM, the shocks play the role of supernova remnant shocks and the core represents the ionized interstellar medium. We consider the effects of both preexisting and selfgenerating magnetic fields and study the evolution of the system by means of twodimensional numerical simulations.
We find that the evolution of the turbulent core is generally, subsonic with rmsMach number . We observe an isotropic, turbulent velocity field with an inertial range power spectra of . We account for the effects of selfmagnetization and find that the resulting magnetic field has characteristic strength G. The corresponding plasma is about , indicating that the magnetic field does not play an important role in the dynamical evolution of the system.
The natural extension of this work is to study the system evolution in threedimensions, with various laser drive configurations, and targets with shells and cores of different masses. The latter modification may help to increase the turbulent intensity and possibly create transonic turbulence. One of the key challenges is to obtain transonic turbulent conditions in a quasisteady state environment.
keywords:
hydrodynamics, turbulence, magnetic fields, laboratory astrophysicsThe main physics processes describing the evolution of the interstellar medium (ISM) are hydrodynamics, magnetization, and radiation processes such as ionization. In addition, the stars are localized sources of mass and energy, some of them, such as supernovae, are very powerful and capable of shaping the evolution and structure of the ISM on global scales. Those interactions eventually result in smallscale structures, including supersonic turbulence.
Absorption and emission at infrared and radio wavelengths are the primary messengers for turbulence in the interstellar medium (ISM). Observations have shown that velocity dispersion is correlated to region size via a power law dependence from subparsec to kiloparsec scales Larson (1979, 1981); Ossenkopf and Mac Low (2002). Observations of velocity and density are consistent with supersonic turbulence driven on large scales (at or above the size of molecular clouds), and exhibit velocity structures indicative of a shockdominated medium Ossenkopf and Mac Low (2002). There is further evidence that smallscale driving from star formation is negligible Brunt and Heyer (2002a, b); Brunt et al. (2009), and the observational velocity scaling is inertial. Radio scintillation measurements provide direct evidence for turbulence on smallscales ( cm) Rickett (1990); Boldyrev and Gwinn (2003).
The existence of supersonic (compressible) turbulence plays an important role in star formation Mac Low and Klessen (2004); Krumholz and McKee (2005); Padoan and Nordlund (2011), the stellar initial mass function Padoan and Nordlund (2002); Hennebelle and Chabrier (2008, 2009), and more fundamentally, the density and velocity statistics of the ISM Elmegreen and Scalo (2004); Scalo and Elmegreen (2004); McKee and Ostriker (2007). The primary metric in these analyzes is the dependence on the density variance with the rms Mach number; for lognormal distributions of the density contrast (), the density variance is given by , where is related to the energy injection mechanism Kritsuk et al. (2007); Lemaster and Stone (2008); Padoan and Nordlund (2011); Molina et al. (2012). Despite analytical Padoan and Nordlund (2011); Molina et al. (2012) and numerical Ostriker et al. (2001); Lemaster and Stone (2008) investigations, the effect of magnetic fields on the density variance remains unclear.
Information about the magnetic field in the ISM can be inferred via Faraday rotation and polarization of synchrotron radiation Troland and Crutcher (2008); Crutcher et al. (2009). Observations based on Zeeman measurements indicate that magnetic effects may play an important role in hydrodynamic evolution Crutcher (1999). However, the sustenance of the interstellar magnetic field may be be coupled to turbulence via generation due to folding and stretching of the field, resulting in smallscale dynamo effects Schekochihin et al. (2004).
Earthbound methods for investigating turbulence in the ISM have come only from numerical modeling. Numerical simulations indicate that the webbed structure of the ISM may result from the nonlinear advection operator Scalo et al. (1998). Additionally, pure hydrodynamic simulations reproduce similar behavior Kritsuk et al. (2007). Marginal quantitative differences are found between hydrodynamic and magnetohydrodynamic simulations when subjected to a background magnetic field de Avillez and Breitschwerdt (2005); however, filaments tend to orient along magnetic field lines. There is numerical evidence that energy transfer between spatial scales may be regulated by shocks, as opposed to a turbulent cascade Lemaster and Stone (2009).
While turbulence has been studied extensively in fluids Frisch, U. (1995); Kellay and Goldburg (2002); Boffetta and Ecke (2012), it has not received the same treatment for plasmas. However, advancements in highenergydensity physics (HEDP) experiments may provide a way to investigate properties of the ISM in the laboratory. Laser systems at the Omega Laser Facility and the National Ignition Facility provide the ability to deposit kilojoule to megajoule energies on the surface of millimeter scale targets over a timescale of picoseconds to nanoseconds. Experimental approaches to potential turbulence inducing effects from RayleighTaylor, KelvinHelmholtz, and RichtmyerMeshkov instabilities have been summarized in Drake et al. (2008a). Replication of turbulence in the ISM will require long driving times, implying the need to drive large amounts of material (large volumes) presumably using multiple blast wavelike impulses created by an array of laser beams.
An initial experimental design to study compressible turbulence in the laboratory was proposed by Drake et al. (2008b). In this design, a gasfilled target box is embedded in a medium. As this surrounding medium is exposed to laser energy deposition, small holes in the box allow driven material to enter the cavity. The interactions of these focused blast waves are then expected to produce turbulent behavior in the interior of the container.
In this work we present a preliminary highenergydensity experimental scenario to investigate shock generated turbulence. Our initial, twodimensional scenario focuses on stirring a target composed of concentric, circular layers with blast waves generated from laser irradiation. We include the effects of magnetic fields in this work by considering three cases; pure hydrodynamics, a preexisting magnetic field, and a magnetic field generated from the Biermann battery source term. Section 1 outlines our experimental design and the corresponding computational model, with supplementary material found in A. Section 2 provides a comparison between the three magnetization cases. Section 3 offers an indepth analysis of the selfgenerated magnetic field case. Discussion and conclusions are offered in Section 4
1 Design, model, & methods
1.1 Experimental scenario
Our preliminary experimental design is based on two concentric spheres as illustrated in Fig. 1. The inner sphere (core) is composed of low density material and provides a medium for the driven mixing process. The outer sphere (shell) is of higher density. The target is embedded in a very low density ambient medium (essentially vacuum). All materials are initially in pressure equilibrium. The aim of this work is to produce an initial investigation of the twodimensional problem.
In order to reproduce a multiply shocked section of interstellar medium, the shell layer is irradiated on its surface by a set of laser drives. The driveshell interactions result in pressure and material waves propagating toward the center of the target. As the shocks pass through the core at different times complex hydrodynamic conditions are created. The primary purpose of the high density shell is to absorb the laser drive and convert thermal energy into kinetic energy. As a result, the perturbations reaching the core region should be kinetically dominated. Our hope is repeated exposure of the shell material to laser pulses should produce a proxy for the effects of supernovae in the ISM. Ideally, the laser system would be arranged in a spherically symmetric configuration to help confinement of the target material and allow for longer evolution of the shocked system.
The effects of laser driving on the shell material is a transient problem that is not of particular interest in this work. We are primarily interested in the effects of mixing in the light core, and therefore consider a “turbulent core” (TC) encompassing the target core and part of the shell. Consequently, we view the area exterior to the TC as generating the boundary conditions for the interior of the TC. The results of this work focus only on data interior to the TC, unless otherwise stated.
1.2 Computational model
We assume that the laboratory setting can be modeled via the extended magnetohydrodynamic equations outlined in Braginskii (1965); Nishiguchi (2002):
(1) 
(2) 
(3) 
(4) 
where , , , , are the fluid density, thermal pressure, specific total energy, material velocity, and magnetic field, respectively. The electron pressure and electron density are denoted by and , respectively. The leading constants on the bracketed term of Eqn. 4 are the speed of light () and electron charge ().
Equation 4 describes the evolution of the magnetic field using the generalized Ohm’s law, where the bracketed term indicates the components that result in selfgeneration of the magnetic field. The first term inside the brackets is the Biermann battery term, and causes field generation when the temperature and density gradients are misaligned. The second term is the Hall term, and indicates that preexisting fields can self amplify. When no initial magnetic fields exist, the Biermann battery term may begin creating a field, which the Hall term will then act upon. We do not include the electronion friction term in our models.
We utilize an ideal gas equation of state with . The plasma composition is represented with a single species with atomic mass, , and atomic charge, . Accordingly, the ion number density is , where is the Avogadro constant. To obtain the electron number density, , we use the ThomasFermi equation of state Salzmann, D. (1998). The required electron number density is calculated as .
1.3 Proteus
The set of Eqns. (1)(4) are solved numerically using the finite volume Proteus code, which is our developmental fork of the FLASH code Fryxell et al. (2000). In this work we use the unsplit staggered mesh solver of Lee, D. and Deane, A.E. (2009). This magnetohydrodynamics (MHD) solver is a variant of the constrained transport method Evans and Hawley (1988) and is used for all cases considered. The MHD solver is formally secondorder accurate in space and time.
The method used for driving the turbulence in these models (Sec. 1.5) produces numerical difficulties for many Riemann solvers. In order to maintain a robust simulation environment, we use the HartenLaxvan LeerEinfeldt (HLLE) Riemann solver Einfeldt (1988).
Computations are performed on a square, Cartesian domain with sides of length 9000m . This allows for the entire target to be placed inside, with additional room to develop in the ambient medium. We treat the boundary conditions as open outflows. While we limit our analysis to the smaller region of interest surrounding the core, simulation of the complete target allows for the interaction of laserdriven material. As the area exterior to the TC can be viewed as boundary conditions for the TC, it is possible that these interactions could affect our results and are accounted for as much as possible.
We utilize statically refined Cartesian meshes for our domain decomposition. We refine the grid inside of the region of interest to a uniform spacing. We perform each case on three separate TC grid sizes: 16m for the coarsest run; 8m for the medium resolution run; and 4m for the fine resolution run. Exterior to the TC we allow the mesh to coarsen radially (subjected to proper nesting). The coarsest cell resolution for all computed models is 64m .
1.4 Initial conditions
gcm  

gcm  
gcm  
bar  
m  
m  
m  
K 
We consider three distinct magnetization cases in this work: pure hydrodynamics; a preexisting, out of plane magnetic field; and selfgenerated magnetic fields (no preexiting field). The pure hydrodynamics case provides a reference from which to gauge the impact of magnetic fields on the flow structure. With these three cases, we aim to begin quantifying the effects of turbulence in high energy density conditions, attempting to include increasing levels of physical complexity. Table 1 shows the shared conditions for all of our models.
The preexisting magnetic field case consists of an initial magnetic field whose only nonzero component is out of the plane. This field provides an additional pressure component (in the form of magnetic pressure), without forcing the advection of material to be along field lines. Such a configuration is difficult to realize in the laboratory, and should be thought of as a toy model. However, it allows us to gauge any magnetic effects in a controlled manner, where we have an a priori estimate of the plasma . (For the entirety of this work we define as .) In order to initialize the magnetic field we use a characteristic reference pressure of bar and choose to solve for the magnitude of the initial magnetic field. Our chosen reference pressure is characteristic of conditions in the turbulent core during the laser driving period, and should put our preexisting field simulations near .
1.5 Shock generation
The requirement of producing highenergy density turbulent plasma in a state close to steady state and as isotropic as possible imposes certain restrictions on the laser drive. In a viable design it would be highly desirable that average linear and angular momenta of the system are close to zero. One possible way to achieve this is to compensate for the linear momentum injected by any laser pulse using a some combination of remaining laser pulses. For example, one could fire two laser beams from opposite directions. This configuration, however, would not allow for lasting plasma confinement. Therefore, a more complex setting is needed, such as a triple (with laser beams originating at the tips of an equilateral triangle in 2D) or a quadruple (with laser beams originating at the tips of a tetrahedron in 3D) laser drive configuration. Furthermore, one would wish to add a certain degree of randomness to the drive in order to promote the development of turbulence. (Although such a drive configuration cannot be realized at existing HEDP laser facilities, our primary goal is to assess the feasibility of possible future designs for turbulent plasma experiments.)
In our twodimensional study, the laser drive configuration is defined by a set of three lasers arranged 120 apart (a triple) in order to improve confinement. Over the course of driving we sample 100 triples every 2 nanoseconds with each laser in the triple fired at the same time. Each triple is offset by a random angle, , sampled from a uniform distribution over . The initial triplet has an angular offset of in order to avoid initial grid symmetries.
While we use Proteus to evolve the target, we do not use it to simulate the lasertarget interaction. Instead, we precompute a twodimensional “laser drive profile” (LDP) and then map it onto the Proteus mesh when a triple is activated. The LDP is a fixed time, two dimensional, cylindrical set of primitive variables, and is further described in A. When mapping the LDP to the Proteus mesh, we place the inward moving tip along a circle of radius m , with the angle of the LDP axis given by the sampled angle .
We note that the process of mapping the LDP onto the Proteus mesh is not conservative. We feel this approach is justified, as the drive is mapped away from the TC, which is an open system in its own right. Thus, the area outside is of ancillary importance in terms of conservation. This method also enables dramatically faster turnaround on model generation, as we do not have to compute lasertarget interactions in the complex media surrounding the TC. More realistic studies aimed at evaluating specific laboratory experiments may have to abandon the LDP concept and compute the laser energy deposition along with the interior calculations at the significant increase of computational time. Again, our aim in this work is to provide initial insights into the behavior of such an experiment.
2 Effect of magnetic fields on hydrodynamics
2.1 Compressibility effects
In order to judge the effects of compressibility, we consider the evolution of the rmsMach number, , shown in Fig. 2 for the hydrodynamic, preexisting field, and selfgenerated cases. The first laserdriven shocks penetrate the low density core at ns, causing a sharp rise in . By ns the core has been completely overrun and the rmsMach number reaches a quasisteady value of approximately 0.2.
For the remaining ns of evolution, continual driving via laser triplets stirs the region of interest. Over this period the rmsMach number marginally decays due to the combined effects of suppressed material accelerations (resulting from the confinement via the laser arrangement) and sound speed increase via compression. During this driving phase there is no discernible effect from either a priori or in situ magnetic fields. The low rmsMach numbers obtained during the driving phase indicates that we are not reaching the supersonic regime. When laser driving ceases at ns there is a marked increase in the rms Mach number. This trend peaks at ns, after which decays to a nominal value of 0.25.
After the laser drive turns off, there is no confining ram pressure to balance the thermal pressure in the core. This results in outward expansion which simultaneously increases material velocity and decreases sound speed. The Mach number is able to stabilize at later times as conditions in the region of interest homogenize. We note that the deviation between and the densityweighted turbulence Mach number is approximately 3% during the driving phase.
2.2 Magnetic field evolution
While magnetic fields do not appear to play a role in the hydrodynamic development of the driven system, the role of generation and amplification in this driven turbulence scenario is interesting in its own right.
The evolution of the magnetic field strength and plasma for the two magnetized cases is shown in Fig. 3. For the case of a weak preexisting magnetic field with , the initial magnitude of the magnetic field G. During the driving phase the field is amplified by a factor of 2, with a mean field strength of G. The distribution of field strength is roughly Gaussian during this period with a negative skew. The cessation of laser driving results in the distribution narrowing and the field strength decaying as the magnetic field is advected from the turbulent core.
The selfgenerating case quickly reaches its peak shortly after the TC is overrun by the first shocks and produces field strengths on the order of G. The resulting field distribution is also a negative skew nonGaussian. Unlike the preexisting case, the shape of the distribution remains static postdriving. However, this distribution undergoes a shift as the magnetic field decays at the same rate regardless of field strength.
The plasma distribution for the preexisting case predominantly covers the moderatetoweak field range of , which agrees with our initial magnetic field estimate of . This distribution contains fluctuations in the larger region and remains roughly constant for smaller. In the postdriving phase decreases to a uniform value on the order of 10 throughout the domain.
In contrast, the distribution for the selfgenerating case maintains the same structure throughout the driving phase, much like the distribution of . The bulk of the distribution is in the range of , indicating very weak effects on hydrodynamics due to the magnetic field. After driving increases drastically in contrast to the preexisting field case.
Figure 4 shows the probability distributions of the magnetic field magnitude with respect to the density and gradient of density. For the preexisting field case, there is a linear correlation between the magnetic field strength and the density. For compressible flows, this is indicative that the compression of the fluid is also compressing the field lines. In contrast, no correlation is seen between the density and field strength for the selfgenerating case. This does not indicate an absence of field line compression, but rather the complicated physics involved with generation hides such a correlation. Preliminary investigation into dependence for the selfgenerated case shows that short term, strong field events occur (on the order of megagauss), but it is difficult to quantify such behavior with the available data. We recommend further work in this area, with a focus on Lagrangian particle analysis.
3 Hydrodynamic evolution of the selfgenerated case
3.1 Morphology
Pseudocolor plots of the density in the region of interest at multiple times is depicted in Fig. 5. At ns the initial laserdriven shocks have penetrated the light core material. The small triangular region at the center of the TC is still unshocked and the preheated region in front of the hydrodynamic shocks can be seen. There are no discernible fluid instabilities at this time, although at previous times small RayleighTaylor and KelvinHelmholtz instabilities could be seen before being overrun by later shocks. The interaction of initial shocks has compressed the triple point areas by a factor of 13 from the shell density.
In the middle of the driving phase ( ns) confinement due to the laser arrangement results in a dense core embedded in a lower density medium. The flow structure appears very chaotic, with the multitude of shocks passing through the core clearly visible. This image is representative of the remaining 70 ns of driving.
At the peak of the postdriving phase (230 ns), the density field exhibits interesting flow features. In particular, there appears to be low density bubbles embedded in the more dense remnant of the core. We note that the maximum density has decreased by a factor of nearly 6 from the snapshot at ns. The bulk distribution of density appears (visually) to be quite anisotropic, with a low density imprint at 120, 220, and 320. Note that the last laser triplet was fired nearly ns prior, and the resulting shocks have left the domain already.
3.1.1 Isotropy
The amount of physical material available in the experimental setting is limited due to the balance between target size and available driving energy. Consequently, confinement of the shocked plasma in the region of interest is of great benefit to the experiment. Therefore, we investigate the isotropy of the velocity field over time, with the most beneficial outcome being that the velocity evolves to a fully isotropic state where the bulk momentum is zero. Additionally, isotropy of the flow field has additional implications for turbulence and the application of Kolmogorov theory.
Probability density contours of the velocity components in the region of interest are shown in Fig. 6. The axes are scaled by the maximum instantaneous velocity magnitude to standardize the figures. The inset shows the angular probability distribution mapped to polar coordinates with the solid line. A fully isotropic distribution is shown with the dashed circle.
As flow features (such as shocks) penetrate the TC and evolve, large velocity gradients are formed. This behavior is reflected in velocity space by tightly packed isocontours. Additionally, the velocity within fluid structures has relatively mild gradients, leading to high probability regions. Therefore, the distribution of isocontour lines is a direct result of the fluid structures inside of the region and one can infer information about the aggregate behavior of flow features in the domain.
At ns three “ejecta” can be seen extending from the origin. In physical space this corresponds to the three dense, multiply shocked regions in Fig. 5. This distribution is highly anisotropic, which is illustrated in the inset. Note that the inset probability plot is rotated by 180 from the apparent position of the shocks because it is a representation of the direction of motion, not position.
In the middle of the driving phase ( ns), the core has been overrun repeatedly with shocks and the chaotic motion induced by the laser driving results in a much more isotropic distribution of velocities shown in the inset. The circular banding of isocontours around the origin implies that flow structures are causing a roughly isotropic distribution of velocity gradients. This indicates that the shocks (in particular, their normals) are isotropically distributed throughout the domain, as the primary source of acceleration in this system comes from the kinetic, laserdriven material (since magnetic field effects play a minor role).
The final snapshot at ns illustrates that the velocity components have begun to fill out the velocity space. There are strong, localized flow features that result in directionally biased velocities; however, the bulk of the distribution remains isotropic. The localized features are the result of the final shocks passing through the domain. The bulk outward motion is due to the lack of laserdriven confinement which allows for pressure gradients to drive material away from the origin.
3.2 Flow field structure during driving
Additional information can be obtained about the flow field during the driving phase by decomposing the velocity into constituent components. Using the Helmholtz theorem Arfken and Weber (2005), we can reformulate the velocity field as , where , , and are the compressive, solenoidal, and harmonic components, respectively. We do not consider the harmonic component in our analysis as it exists only as a correction for nonperiodic domains and plays no dynamical role in the system. In order to compute these terms, we rewrite them in terms of their Fourier transforms,
(5) 
(6) 
Equations 5 and 6 are easily computed and inverted to produce the corresponding velocity fields in physical space. Additional details of our computations involving the Fourier transform are found in Sec. 3.2.3.
Figure 7 shows streamlines of the velocity field and its components at ns for a square subsection of the region of interest. The left most image shows the streamlines for the total velocity field ().
The middle image illustrates the compressive component of the velocity field (). The sources and sinks in the field are now clearly visible. The pointlike areas where streamlines fan out are indicative of the expansion of material ().
The domain is also populated by “line sinks” where streamlines abruptly end along a curve. These features are regions of fluid compression (), induced by either strong perturbations or weak shocks. Strong shocks in the domain are rare, and the flow field is predominantly populated by strong perturbations.
The final set of streamlines are for the solenoidal component of the velocity field (). One can easily identify the underlying vortical structure of the flow field now. In particular, the domain consists of nested vortices typical of turbulence. As we are dealing with two dimensional turbulence, it is conceivable that the small vortices induce the larger structures due to the inverse enstrophy cascade. For the subsection pictured, the largest cell is approximately 1600m in diameter, while the smallest cell contained within has a diameter of roughly 100m .
3.2.1 Radial distribution
Figure 8 quantifies the descriptions provided in Sect. 3.1, showing density and pressure as a function of distance from the center of the target. These results are obtained by constructing probability distribution functions for grid cells contained in circular shells of 50m width. Thick solid lines denote the mean value while thin solid lines show the minimum and maximum values.
During the middle of the driving phase ( ns), the density peaks at m away from the core, and decays as the radius increases. The pressure is relatively low at the center of the core, and increases until m when it peaks and decays slightly.
By the time the laser drives cease firing at ns, the density profile has flattened near the core, but continues to decay with radius. The pressure near the center of the core has increased, bringing the region of interest into approximate thermal equilibrium.
At ns, at the peak of the rmsMach number, the average density profile in the core has homogenized, staying roughly constant out to m . Note that the maximum mean density has decreased by approximately a factor of 4. While the pressure profile indicates that the region is still roughly in thermal equilibrium, the mean value has decreased by an order of magnitude.
3.2.2 Density probability distribution functions
In addition to investigating the spatial dependence on density, we can also look at the probability distributions in the region of interest. Figure 9 shows these distributions during and after the driving phase for the selfgenerating case. Comparing the distributions at early and late times during driving, we note that the profiles are generally similar and follow lognormal distributions with parameters , for the ns distribution, and , for ns. These long tails are the byproduct of shockdriven turbulence. The latetime distribution also indicates that mass has been added to the region from the driving, but this was to be expected due to the nature of the open system.
The postdriving distribution of density is quite different from that of the driving phase. It has become strongly bimodal and no longer exhibits the extended tail that characterized the driving phase distributions. In addition, the densities have shifted to lower values with the low and high density peaks at approximately g cm and g cm, respectively. This result quantifies the structures at late times shown in Fig. 5.
3.2.3 Kinetic energy power spectra
In order to compute the velocity power spectra on the mesh we consider a square area of 1000m by 1000m inside the region of interest. Our finest mesh (4m resolution) provides a uniform grid. Likewise, the 8m and 16m meshes produce and grids, respectively. From these grids we compute the numeric Fourier transform of , , using the fast Fourier transform. We define the multifrequency, total velocity power spectra as . In order to reduce this to a function of a single, mean wavenumber we average over circular shells of unit thickness in space. In addition to the spectrum for the total velocity field, we also examine the power spectra for the compressive and solenoidal components of the velocity field, and .
Figure 10 shows estimated velocity power spectra at ns, ns, and ns for the 4m resolution, selfgenerating case. Figure 11 shows the evolution of the power law exponent, , for the total, solenoidal, and compressive components. A leastsquares fit over the range is used to estimate . The profiles are smoothed over a ns window to remove high frequency oscillations and allowing differentiation of the curves.
In all snapshots the inverse energy cascade () is visible up to the driving mode at .
During the driving phase, the power spectra in the inertial range () scales as . This behavior is similar to the classical theory of magnetohydrodynamic turbulence, where two dimensional behavior obeys Kraichnan (1965); Kraichnan and Montgomery (1980). This relation is likely coincidental as the magnetic field in these two dimensional simulation is generated outofplane and acts only as an additional pressure term. The selfgenerated magnetic fields produce negligible pressures that are unable to drive material motion over the timescales considered. Indeed, these results agree with the same analysis run on the pure hydrodynamic case. As a result, the deviation from the expected behavior is most likely due to the laserdriven stirring.
In the postdriving phase the behavior of the compressive and solenoidal power spectra diverge. The equilibration of pressure in the region of interest results in a substantially weaker contribution from compression effects. In the absence of inertial forces, the dominant process is the interaction between vortical cells. This makes the system appear diffusiondominated rather than advectiondominated. This has certain consequences on the kinetic energy spectra, causing it to assume the form (Fig. 11, ns). This can be explained by transforming the diffusion operator into space, which gives a timeindependent spectra with dependence.
We note that it is typical to see the inertial region smoothly transition into numerical dissipation at high wave numbers. However, the inertial region flattens before abruptly dropping into the dissipation range (not shown is a smoothly decaying knee beginning after the sudden drop). We believe there are two possible causes for this bottleneck effect.
A potential physical explanation is that the stirring mechanism limits the cascade of energy to smaller scales. In particular, shocks moving through the turbulent core will overrun and destroy smallscale features. As such, the driving process may impose a lowerlimit on feature size resulting in a buildup of power near this lower bound.
An alternative explanation for the bottleneck is that numerical effects halt the transfer of energy to smaller scales Sytine et al. (2000). As we were unable to successfully compute models using Riemann solvers other than HLLE, this hypothesis is difficult to either confirm or refute.
4 Discussion and conclusions
We have presented the results of a computational study of a highenergy density physics laserdriven experiment aimed at producing supersonic turbulence in plasma. The design included a target irradiated by sets of laser beams to provide plasma confinement and induce turbulence. To this end we computed a generic laser drive profile (LDP). During the evolution, the LDP has been mapped at select positions and times in such a way as to create turbulent conditions in the central region of the target.
We found that:

The turbulence Mach number reaches nominal, quasisteady value of 0.2 throughout the driving phase for all cases. There is a minor downward trend as the material in the turbulent core is increasingly thermalized. Shortly after the driving phase, the turbulence Mach number rises due to the conversion of suppressed thermal energy into kinetic energy as the confining ram pressure is removed. In the postdriving phase the turbulence Mach number reaches steady values of about 0.25.

The magnetic fields produced for the outofplane a priori field are on the order of megagauss. These fields correspond to . Amplification of the magnetic field due to driving results in a factor of 2 increase during the driving phase. In the postdriving phase the spatial distribution becomes uniform with a nominal value on the order of 100 kG.
The selfgenerated magnetic fields obtain kilogauss strengths during the driving phase. These fields correspond to , indicating that the effects due the magnetic field on the hydrodynamic development of the system are minimal.

The distribution of material velocity obtains an isotropic distribution during the driving phase for the selfgenerated case.

The velocity power spectra show the expected inverse energy cascade and forward enstrophy cascade during the driving phase. The forward enstrophy cascade obeys in the inertial range (). The deviation from the twodimensional, hydrodynamic behavior of is due to the laserdriven mechanism and not magnetic field effects.

The solenoidal and compressive kinetic energies are roughly in equipartition during active driving. In the postdriving phase, the solenoidal component contains the bulk of the kinetic energy (with a ratio on the order of 100:1).
We conclude that, in principle, one can produce a weakly compressible, quasisteady state, turbulent plasma in laser driven experiments for as long as driving is provided. We note, with some disappointment, that the particular choice of parameters did not produce supersonic turbulence. We found this primarily due to the turbulent central region being filled with the ablating material. It would be interesting to consider a scenario in which the entire target is composed of a single material. In the case that the target is made out of the low density material used in this study, one could expect the turbulent Mach number to increase by a factor of (2.2).
Furthermore, it is conceivable that by adjusting the firing frequency of the laser, and the energy and pulse length of individual beams one can change the thermodynamic conditions in the turbulent core. This provides a way to control the sound speed, and therefore the turbulent Mach number opening a possibility of reaching the supersonic regime.
One aspect of the proposed design we did not discuss in this work in detail is experimental diagnostics. We defer the discussion of this crucial component of the experiment until more realistic computations are performed in threedimensions.
5 Acknowledgments
TH and TP were supported in part by the DOE grant DEFG5209NA29548 and the NSF grant AST1109113. The authors wish to thank Mike Grosskopf of the University of Michigan for his assistance with configuring the CRASH code. This research used resources of the National Energy Research Scientific Computing Center, which is supported by the Office of Science of the U.S. Department of Energy under Contract No. DEAC0205CH11231. The software used in this work was in part developed by the DOE Flash Center at the University of Chicago.
Appendix A Calculation of the Laser Drive Profile
We compute the laser drive profile (LDP) using the CRASH code van der Holst et al. (2011). In this configuration, a 2.5D cylinder of carbon foam is irradiated along the positive axis. The physical domain for the LDP simulations is m m , and m . The initial density is set to for , and for . Initially, both layers are in pressure equilibrium at Pa. These conditions match those of the target in the full Proteus simulation. The LDP simulations do not contain any magnetic field effects.
The incident irradiation is defined by by a superGaussian laser beam of order , with a standard deviation of m in the radial direction, and whose center is coincident to the axis of symmetry. The pulse is a constant W for ns with a linear rise and decay time of ns. Laser energy deposition is accomplished using CRASH’s geometric raytracing functionality with individual rays representing the beam.
We performed two runs with uniform mesh resolutions of m and m . These resolutions are at least a factor of two smaller than the Proteus mesh the LDP is mapped to. We determined there were minimal differences between the two resolutions.
We choose the evolutionary snapshot to be used as the LDP by finding the moment when the rarefaction fan catches up to the shock front. The laser driven flow is thermally developed at this point, and the bulk of the energy transferred to the shell will be in the form of kinetic energy. This corresponds to the snapshot at ns in both the m and m simulations. This evolutionary time is after the CRASH laser drive turns off and we are not truncating any laser physics by choosing the ns snapshot.
Depicted in Fig. 12 are the pseudocolor plots for density, thermal pressure, and velocity magnitude. The laser drive produces a parabolic structure moving predominately in the radial direction. By the time the flow becomes thermally developed the extent the blast wave reaches nearly m . The ablation near the beam leaves a low density, high pressure region behind the shock, implying that the bulk of the kinetic energy that will reach the core is compressed near the shock structure. In addition, the model shows a substantial preheat region ahead of the shock.
The only qualitative difference between the m and m models is near the symmetry axis; the m model shows a slightly more bulbous structure. We do not think this will affect the generation of turbulence. Therefore, in the interest of memory constraints and mapping time, we choose to use the m model as the prototypical laser drive.
a.1 Mapping the laser drive profiles
We interpret the configurations described in Sec. 1.4 as a set of cylinders (rectangles in twodimensions) embedded into the shell of the target. The geometry of these cylinders are computed at code startup on each processor. Additionally, LDP hydrodynamic variables (obtained in Sec. A) are loaded onto each core.
When it is decided that a laser should be fired in the Proteus simulation (described in Sec 1.4), the cells owned by a processor are searched to determine if any reside inside, or are clipped by, the laser cylinder. If any do, the location of the cell in the cylinder’s local coordinate system are determined. From this information, we determine where the cell lies in the twodimensional CRASH data set. In the case of two dimensions, this is intuitive as we are rotating and shifting a rectangle onto another rectangle. In three dimensions we only consider the axial and radial coordinates in the cylindrical coordinate system, and discard the angular component. In our study this is reasonable, as we are mapping an axisymmetric data set. However, we note that mapping a threedimensional data set into the cylinder (or any other geometric primitive) requires a physically meaningful definition of the rotation about the axis, complicating the modeling of the system.
After determining our current cell’s position in the data set frame, we interpolate the data set quantities using bilinear interpolation. In order to enhance the mapping obtained, we perform the interpolation on a uniform grid of 10 points per dimension, weighting by subcell volume.
The quantities interpolated from LDP are forcibly written onto the mesh in the precomputed location. This entails overwriting the values of density, pressure, and velocity components (transformed into the coordinates of the cylinder axis). We lessen obtrusiveness of mapping on the surroundings by only using the LDP data inside of a pressure cutoff of Pa. This cutoff is shown as the gray or black solid line moving through the domain in Fig. 12. Additionally, strong discontinuities near the edge of the mapped data can lead to failures of the Riemann solver. To circumvent this problem we smooth the fields with an arithmetic averaging filter of cells near the edge.
References
 Larson (1979) R. B. Larson, Mon. Not. R. Astron. Soc. 186 (1979) 479–490.
 Larson (1981) R. B. Larson, Mon. Not. R. Astron. Soc. 194 (1981) 809–826.
 Ossenkopf and Mac Low (2002) V. Ossenkopf, M.M. Mac Low, Astron. Astrophys. 390 (2002) 307–326.
 Brunt and Heyer (2002a) C. M. Brunt, M. H. Heyer, Astrophys. J. 566 (2002a) 276–288.
 Brunt and Heyer (2002b) C. M. Brunt, M. H. Heyer, Astrophys. J. 566 (2002b) 289–301.
 Brunt et al. (2009) C. M. Brunt, M. H. Heyer, M.M. Mac Low, Astron. Astrophys. 504 (2009) 883–890.
 Rickett (1990) B. J. Rickett, ARA&A 28 (1990) 561–605.
 Boldyrev and Gwinn (2003) S. Boldyrev, C. Gwinn, Astrophys. J. 584 (2003) 791–796.
 Mac Low and Klessen (2004) M.M. Mac Low, R. S. Klessen, Reviews of Modern Physics 76 (2004) 125–194.
 Krumholz and McKee (2005) M. R. Krumholz, C. F. McKee, Astrophys. J. 630 (2005) 250–268.
 Padoan and Nordlund (2011) P. Padoan, Å. Nordlund, Astrophys. J. 730 (2011) 40.
 Padoan and Nordlund (2002) P. Padoan, Å. Nordlund, Astrophys. J. 576 (2002) 870–879.
 Hennebelle and Chabrier (2008) P. Hennebelle, G. Chabrier, Astrophys. J. 684 (2008) 395–410.
 Hennebelle and Chabrier (2009) P. Hennebelle, G. Chabrier, Astrophys. J. 702 (2009) 1428–1442.
 Elmegreen and Scalo (2004) B. G. Elmegreen, J. Scalo, ARA&A 42 (2004) 211–273.
 Scalo and Elmegreen (2004) J. Scalo, B. G. Elmegreen, ARA&A 42 (2004) 275–316.
 McKee and Ostriker (2007) C. F. McKee, E. C. Ostriker, ARA&A 45 (2007) 565–687.
 Kritsuk et al. (2007) A. G. Kritsuk, M. L. Norman, P. Padoan, R. Wagner, Astrophys. J. 665 (2007) 416–431.
 Lemaster and Stone (2008) M. N. Lemaster, J. M. Stone, Astrophys. J. 682 (2008) L97–L100.
 Molina et al. (2012) F. Z. Molina, S. C. O. Glover, C. Federrath, R. S. Klessen, Mon. Not. R. Astron. Soc. 423 (2012) 2680–2689.
 Ostriker et al. (2001) E. C. Ostriker, J. M. Stone, C. F. Gammie, Astrophys. J. 546 (2001) 980–1005.
 Troland and Crutcher (2008) T. H. Troland, R. M. Crutcher, Astrophys. J. 680 (2008) 457–465.
 Crutcher et al. (2009) R. M. Crutcher, N. Hakobian, T. H. Troland, Astrophys. J. 692 (2009) 844–855.
 Crutcher (1999) R. M. Crutcher, Astrophys. J. 520 (1999) 706–713.
 Schekochihin et al. (2004) A. A. Schekochihin, S. C. Cowley, S. F. Taylor, J. L. Maron, J. C. McWilliams, Astrophys. J. 612 (2004) 276–307.
 Scalo et al. (1998) J. Scalo, E. VazquezSemadeni, D. Chappell, T. Passot, Astrophys. J. 504 (1998) 835.
 de Avillez and Breitschwerdt (2005) M. A. de Avillez, D. Breitschwerdt, Astron. Astrophys. 436 (2005) 585–600.
 Lemaster and Stone (2009) M. N. Lemaster, J. M. Stone, Astrophys. J. 691 (2009) 1092–1108.
 Frisch, U. (1995) Frisch, U., Turbulence: the legacy of A.N. Kolmogorov, 1995.
 Kellay and Goldburg (2002) H. Kellay, W. I. Goldburg, Reports on Progress in Physics 65 (2002) 845.
 Boffetta and Ecke (2012) G. Boffetta, R. E. Ecke, Annual Review of Fluid Mechanics 44 (2012) 427–451.
 Drake et al. (2008a) R. P. Drake, E. C. Harding, C. C. Kuranz, Physica Scripta 2008 (2008a) 014022.
 Drake et al. (2008b) R. P. Drake, N. Patterson, K. Thornton, M. J. Grosskopf, N. Hearn, T. Plewa, 11th International Workshop on the Physics of Compressible Turbulent Mixing, 2008b.
 Braginskii (1965) S. I. Braginskii, Reviews of Plasma Physics 1 (1965) 205.
 Nishiguchi (2002) A. Nishiguchi, Jpn. J. Appl. Phys. 41 (2002) 326.
 Salzmann, D. (1998) Salzmann, D., Atomic Physics in Hot Plasmas, Oxford University Press, 1998.
 Fryxell et al. (2000) B. Fryxell, K. Olson, P. M. Ricker, F. X. Timmes, M. Zingale, D. Q. Lamb, P. MacNeice, R. Rosner, J. W. Truran, H. Tufo, Astrophys. J. Suppl. Ser. 131 (2000) 273–334.
 Lee, D. and Deane, A.E. (2009) Lee, D. and Deane, A.E., J. Comput. Phys. 228 (2009) 952.
 Evans and Hawley (1988) C. R. Evans, J. F. Hawley, Astrophys. J. 332 (1988) 659–677.
 Einfeldt (1988) B. Einfeldt, SIAM Journal on Numerical Analysis 25 (1988) 294–318.
 Arfken and Weber (2005) G. Arfken, H. Weber, Mathematical Methods for Physicists, Academic Press, sixth edition, 2005.
 Kraichnan (1965) R. H. Kraichnan, Physics of Fluids 8 (1965) 1385–1387.
 Kraichnan and Montgomery (1980) R. H. Kraichnan, D. Montgomery, Reports on Progress in Physics 43 (1980) 547–619.
 Sytine et al. (2000) I. V. Sytine, D. H. Porter, P. R. Woodward, S. W. Hodson, K.H. Winkler, Journal of Computational Physics 158 (2000) 225–238.
 van der Holst et al. (2011) B. van der Holst, G. Tóth, I. V. Sokolov, K. G. Powell, J. P. Holloway, E. S. Myra, Q. Stout, M. L. Adams, J. E. Morel, S. Karni, B. Fryxell, R. P. Drake, Astrophys. J. Suppl. Ser. 194 (2011) 23.