Critical fluctuations and anomalous transport in soft Yukawa-Langevin systems

Critical fluctuations and anomalous transport in soft Yukawa-Langevin systems

S. Ratynskaia, G. Regnoli, K. Rypdal, B. Klumov, G. Morfill Space-and Plasma Physics, Royal Institute of Technology, Stockholm, Sweden
Max-Planck-Institut für extraterrestrische Physik, Garching, Germany
Department of Physics and Technology, University of Tromsø, Norway
July 17, 2019
Abstract

Simulation of a Langevin-dynamics model demonstrates emergence of critical fluctuations and anomalous grain transport which have been observed in experiments on “soft” quasi-two-dimensional dusty plasma clusters. Our model does not contain external drive or plasma interactions that serve to drive the system away from thermodynamic equilibrium. The grains are confined by an external potential, interact via static Yukawa forces, and are subject to stochastic heating and dissipation from neutrals. One remarkable feature is emergence of leptokurtic probability distributions of grain displacements on time-scales , where is the time at which the standard deviation approaches the mean inter-grain distance . Others are development of humps in the distributions on multiples of , anomalous Hurst exponents, and transitions from leptokurtic towards Gaussian displacement distributions on time scales . The latter is a signature of intermittency, here interpreted as a transition from bursty transport associated with hopping on intermediate time scales to vortical flows on longer time scales. These intermittency features are quantitatively modeled by a single-partice Itô-Langevin stochastic equation with a non-linear drift term.

I Introduction

Since a large aggregate of dust grains embedded in a plasma can attain virtually all known states of matter review (), the ability of optical tracking of individual grain trajectories has made these systems particularly attractive for studying transport properties and emergent complex behavior in soft materials.

In a number of recent dusty plasmas experiments anomalous properties, like non-Gaussian displacement distributions and anomalous diffusion, have been observed. Yet it is not clear whether this behavior derives from non-equilibrium physics due to external forcing of the grain aggregate, or whether critical fluctuations Christensen () and anomalous transport may emerge in aggregates subject exclusively to statically screened Coulomb forces and independent stochastic forcing and friction due to collisions with the background neutral gas. The purpose of this paper is to demonstrate that the latter is possible, and that non-Gaussian statistics does not have to arise from particular non-equilibrium physics.

So far few molecular-dynamics (MD) or Langevin-dynamics (LD) simulations of dust transport have been able to reproduce the anomalous results observed in experiments, although subdiffusion on short time scales have recently been reported for a bidispersive disordered assembley of Yukawa particles Reichardt2007 (). Here we adopt the terminology employed in GoreePRE2008 (), where MD refers to simulation of an aggregate of particles interacting via Yukawa forces and LD refers to a system that in addition is subject to stochastic forcing and friction represented by a Langevin thermostat. The latter represents a heat bath which should allow the system to relax to thermodynamic equilibrium with the neutral gas.

Under ground-based laboratory conditions dust grains levitate in electrostatic sheaths, which give rise to plasma anisotropy and supra-thermal ion flows that may act as external forcing. Such experiments are referred to as two-dimensional (2D or quasi-2D) due to the fact that vertical motion of particles is severely restricted (monolayers) and/or particles are vertically aligned due to the ion flow. Dust transport under such conditions has been extensively studied both in laboratory LinI1998 (); LinI2001 (); LinI2002 (); LinI2004 (); LinIPPCF2004 (); LinIPPCF2005 (); PoP (); PRL (); GoreePRE2007 (); GoreePRL2008 (); GoreePRE2008 (); NPJ (); Knapek () and simulations GoreePRE2007 (); GoreePRL2008 (); GoreePRE2008 (); NPJ (); Knapek (). Anomalous transport exhibiting Gaussian GoreePRE2007 (); GoreePRE2008 () as well as non-Gaussian LinI2002 (); LinIPPCF2004 (); PoP (); PRL (); GoreePRL2008 () statistics has been reported for both 2D and quasi-2D cases.

In this paper we show that a model that includes only Yukawa interaction between particles, an externally imposed confining potential, and stochastic heating and dissipation from neutrals, is able to demonstrate emergence of non-Gaussian statistical features associated with observed cooperative particle hopping LinI1998 (); LinI2002 (); LinIPPCF2004 (); LinIPPCF2005 (); PoP () and vortical flow patterns PRL (); NPJ (). The simulations also reveal some features for which we report the experimental footprint here for the first time - the development of humps on the displacement probability distribution function (PDF) corresponding to integer multiples of the mean inter-grain distance .

We study quasi-2D systems with varying “stiffness”, with particular attention paid to the transition in transport characteristics from time scales to , where is the characteristic time for a dust grain to diffuse a distance , i.e. . For this purpose we analyze data from ground-based laboratory experiments (quasi-2D) and perform molecular dynamics simulations in quasi-2D and 2D over a range of states, from pure crystal to liquid with particular focus on soft (viscoelastic or hexatic) states at the transition between crystal and liquid.

By examining and contrasting these data, the following picture emerges: the shape of the position displacement distribution is Gaussian for times shorter than the grain-grain collision time . On these short time scales the grain motion is ballistic, and the displacement divided by can be interpreted as the instantaneous grain velocity. Hence the Gaussian displacement PDF reflects the Maxwellian velocity distribution resulting from the Gaussian stochastic heating term. On scales the PDF develops a leptokurtic shape. For stiffer systems, as approaches humps develop on the tail of the PDF at displacements corresponding to integer multiples of . These humps signify that on these time scales the grain hopping in the imperfect hexagonal lattice influences the statistical transport characteristics. On even longer time scales, the kurtosis of the PDFs approach that of a Gaussian, indicating that multiple hoppings may represent a sequence of independent transport events LinI2002 ().

In softer systems the picture on intermediate and longer time scales is different. The humps due to hopping are masked by the emergence of large-scale vortical motions, and the PDFs on the hydrodynamical time-scales reflect these vortex motions.

An interesting observation is that Gaussian statistics characterizes both the solidified crystalline state and the pure liquid state. Non-Gaussian statistics appears when the crystal is sufficiently soft to allow development of defects and particle hopping, but sufficiently stiff to restrict free diffusion on scales larger that . It appears on spatial displacement scales from a fraction of and at least up to those scales where elasticity dominates over viscosity. The fact that Gaussian statistics and normal transport is restored in the purely liquid phase, indicates that the anomalous characteristics are associated with critical fluctuations in the form of a scale-free hierarchy of vortices NPJ (). The vortices emerge from the stochastic forcing only if the lattice resides in a soft, viscoelastic transitional state between crystal and liquid.

We also discuss the possible physical origin of non-Gaussian displacement distributions and anomalous transport, and show how these feature derive naturally from a single-particle Langevin equation with a non-linear drift (friction) term modeling the collective effects of dust-dust interaction.

Ii Data sources

Figure 1: (Color online) Grain trajectories from the molecular dynamics simulations of the Yukawa-Langevin system. The trajectories are color-coded by the time. Motion of particles during time in the case of parabolic confinement (a) and the hard wall confinement (b). A typical trajectory from the outer region of panel (a) plotted for time (c). Close-up on stiff central region of panel (b), motion of particles is shown for (d).

ii.1 Laboratory experiments

For this paper a re-analysis has been made of raw data from the experiment reported in Ref. PoP (). This experiment was performed in a capacitively coupled rf discharge operated in argon at pressure 1.8 Pa and rf power of 10 W. A cluster of 120 melamine- formaldehyde monodispersive spheres with a diameter of 8.9 m, was confined by the potential created by a copper ring mounted on the lower electrode. The dust particles were illuminated by a horizontal laser sheet, and 50 000 images were taken by a video camera at a sampling rate of 30 Hz and spatial resolution of 6.7 m/ pixel.

As seen from Fig. 1(b) of Ref. PoP (), where trajectories of particles over time lag of 1.7 sec are presented, the grains have limited mobility, and we refer to these data as our “stiff cluster” experiment. The re-analysis shows the evolution of radial displacement PDFs computed with improved statistics compared to that of Ref. PoP (). This new analysis reveals features of the PDFs which were not resolved in the earlier data, and also allows us to obtain PDFs of displacements on much longer time scales.

In Ref. PRL () a large circular cluster of 600 dust grains in a monolayer configuration was studied in a similar experimental set-up. The cluster was brought to a partly ordered state allowing large-scale viscoelastic vortex flows (see Figs. 1 and 2 of Ref. PRL ()). The experiment was operated in argon at a pressure 4 Pa and rf power of 19 W with melamine-formaldehyde spheres with diameter of 7.2 m. The grains were confined radially by the potential created by a cavity of 6 cm radius machined into the lower electrode. The cluster diameter was 16 mm with interparticle distance mm. In this experiment 30 000 images were taken by a video camera at sampling rate of 30 Hz and spatial resolution of 24 m/pixel. We will refer to this data as the “soft cluster” experiment.

We will also connect the results from our model simulations to the experimental studies on cold quasi-2D dusty-plasma liquids reported in Refs. LinI1998 (); LinI2002 (); LinIPPCF2004 (); LinIPPCF2005 ().

ii.2 Langevin dynamics simulations

The simulations are performed for the Yukawa system of particles embedded into a Langevin thermostat book () which simulates the effect of the collisions with the electrically neutral molecules of the background gas (details are given in MD ()). The pair interaction between the dust particles is described by the Debye-Hückel (Yukawa) potential:

(1)

where is the particle charge and is the the plasma screening length. Particle radius, mass and charge, mean inter-particle distance, neutral gas density and temperature are the parameters of the simulations. Initially particles having the charge are randomly distributed over a prescribed simulation volume to reach a value of (average) screening parameter close to that in the experiments. After a transient phase, the system relaxes to a statistically stationary state with the dust velocity distribution in thermal equilibrium with the Langevin thermostat. This state does not depend on the initial conditions, which is also the case in the experiments. Three-dimensional particle dynamics of the i’th particle with mass evolves according to the equation,

(2)

where is the neutral gas friction, is the confinement potential and . The stochastic Langevin force (thermal noise induced by neutral gas particles) is defined from the relation:

(3)

with the mean zero condition , where is the neutral gas temperature.

Two types of the confinement have been used in the simulations; parabolic and hard wall. For the parabolic trap the confinement potential is . For the hard wall case the electric field associated with the confinement exponentially increases to the boundaries, so that at and for , where is the size of the system and is a stiffness of the hard wall potential. In our simulations a value of has been used.

To simulate a quasi-2D configuration the motion in the vertical () direction has been suppressed by a strong confinement in this direction. In most of the runs performed, the particle displacements were restricted to a range smaller than the mean horizontal interparticle distance , which is the typical situation for monolayer experiments. In addition, simulations of 2D systems (only horizontal - and - components considered) have also been run for both types of the confinement.

The parabolic confinement is in some respects a more realistic representation of the experiments discussed here and, as seen from Fig. 1(a) it reproduces flow fields quite similar to those observed in the experiments. As in the experiment, such confinement results in a nonuniform cluster with more packed and stiff core and looser boundaries. The hard-wall potential, see Fig. 1(b), yields a different structure; particles are more packed at the boundaries (for more details see cnfkl1 (); cnfkl2 (); cnfkl3 ()). Ideally, comparison of these different confinement schemes could help identifying transport features which are robust to variations of the confinement.

As one can observe from Fig. 1(a) the resulting equilibrium state is a cluster of dust grains in a partially ordered (hexatic) phase, similar to those reported from 2D Yukawa MD simulations on square double-periodic domains in e.g. Reichardt2003 () and in 2D hard-core simulations in Zangi (). However, our cluster is of finite size (non-periodic boundary conditions), confined by a circular symmetric parabolic potential, and is radially nonuniform. Like in the experiments the simulations are intended to describe, the transport over large distances takes place through development and propagation of 5-fold and 7-fold topological crystal defects.

By tuning the input parameters we obtain different states, ranging from pure crystal to pure liquid. As mentioned in the introduction we are mainly focused on semi-ordered (viscoelastic) states at the transition between crystal and liquid. To obtain such states, the coupling parameter, defined as , was changed in the range by varying . The latter also implies change of the inter-particle distance; the corresponding range of the screening parameter was , which is typical for the experiments. For each state studied, was determined as the distance to the first local maximum of the pair correlation function averaged over the cluster. This distance varies less than from the core to the edge for parabolical confinement, and is nearly uniformly distributed in space for hard wall confinement.

The particle positions have been sampled with a time resolution chosen to be of the order of grain-grain collision time scale, . The grain-grain interaction time was estimated as , where is the Einstein frequency which characterizes the linear oscillations of individual particles in a lattice and is a function of the screening parameter . For the Einstein frequency is about a factor of two of the dust-plasma frequency Knapek (). The dust-neutral collision time scale was for all runs.

For each state, a simulation of particles has been run during a time , thus proving adequate statistics for study of the system’s evolution on long time scales.

In both experiments and simulations the nature of the dynamics in the regimes where the system is in a semi-ordered state is very sensitive to fine tuning of the control parameters, and we have not been able to reproduce all experimental features quantitatively. One reason for this may be that we are not able to fine tune parameters to the right state, but it can also be due to shortcomings of the model. However, the purpose of this paper is not to reproduce experimental results quantitatively, but to demonstrate that important qualitative features emerge from a simple Langevin model which does not involve other interactions between the dust particles and the plasma than the Debye screening of the Coulomb potential.

Iii Results on grain transport

iii.1 Laboratory results

Figure 2: Experimental results from stiff cluster (Ref.PoP ()). PDFs of radial displacements (dots) in units of interparticle distance, , for different time lags;  s (a),  s (b),  s (c) and  s (d). The full curves are fits of the stretched Gaussian given by Eq. (4) with (a-d), and the thick full curve is a Gaussian fit (d).

Time evolution of the PDFs of radial displacements in units of interparticle distance for the stiff cluster is shown in Fig. 2. The distributions are presented on a logarithmic scale and the deviation from a Gaussian shape on small time scales Fig. 2 (a,b) is evident. On those scales the shape of the PDF is well described by the stretched Gaussian

(4)

where corresponds to an exponential distribution and to the Gaussian. For the data presented the nonlinear fit (thin full lines) yields the exponent .

A possible, and rather trivial, explanation of the stretched gaussian PDFs would be the spatial non-uniformity of the system. For instance, the dust grains in the laboratory clusters are more mobile close to the edge than in the central region. Thus, it is conceivable that a more heavy-tailed PDF could emerge from combining several Gaussian PDFs with different variances. We have tested this in the laboratory data by producing separate PDFs for particle displacements in the core and edge regions, respectively. However, although these PDFs have different variances, they both retain essentially the same stretched-Gaussian PDF, and hence this is an intrinsic property of the particle dynamics on the short scales both in core an the edge, and is not an artifact due to spatial non-uniformity.

When a significant number of particle displacements approach the mean inter-grain distance the PDF starts to develop “shoulders” around (Fig. 2(c)). The transition towards a Gaussian (Fig. 2(d), thick line) on the longest time scales involves a regime where the PDF develops “humps” at , where is a positive integer.

The humps on the PDFs are most easily explained as an effect of grain “hopping” due to defects in the hexagonal crystal structure. The humps can be observed only in relatively stiff systems where the hopping transport is not masked by the fluid vortical motion. This is clearly illustrated if we compare results for the stiff cluster (Fig. 2) with those for the softer cluster. As seen from Fig.  3 of Ref. PRL (), in the latter experiment, PDFs are well described by Eq. (4) with on the small time scales, and a transition to Gaussian shape is observed already at the scales of . On very large scales, , new humps emerge (Fig. 4(a) of Ref. PRL ()) which are due to large-scale vortical motion PRL (); NPJ ().

In other experiments on quasi-2D laboratory dusty plasma similar results have been found. In studies of cold quasi-2D dusty-plasma liquids, Refs. LinI1998 (); LinI2002 (); LinIPPCF2004 (); LinIPPCF2005 () reported non-Gaussian PDFs on scales below . Moreover, we find that the central portion of the PDF presented in Fig. 3 of Ref. LinIPPCF2004 () can be fitted by Eq. (4) with . On longer time scales, when particle diffuse to distances , the PDFs in those experiments approach a Gaussian shape.

In the next subsection we show that the picture descried above is consistent with the results of simulations of the Langevin dynamics model.

iii.2 Langevin dynamics simulation results

Figure 3: (Color online) Langevin dynamics simulation of Yukawa system for the case of hard wall confinement. PDFs of horizontal displacements (dots) in units of , plotted for different time lags as indicated in the upper corner. The full curve in (a) is a Gaussian fit and the full curves in the zoom-in figures (e,f) are fits by a stretched Gaussian given by Eq. (4) with values of as indicated in the upper left corner.

The effect of the hexagonal lattice structure is, as suggested above, most pronounced in the stiffer states. Langevin dynamics simulations with hard-wall confinement potential reveals this quite clearly. In Fig. 3(d) one observes humps on the tail of the distribution up to . Fig. 3(a), shows the PDF of horizontal displacements on time scales , which is close to the collision time scale. On these time scales the grain motion is still ballistic, and the Gaussian PDF reflects the Maxwellian velocity distribution. On longer time scales the core of the distribution develops into a stretched Gaussian (see Fig. 3 (c,d) and zoom-in (e,f)), and shoulders (and later - humps) develop on the tail. These non-Gaussian features are obviously a result of hopping of some grains from one potential minimum in the crystal lattice to another.

It is interesting to compare these PDFs to those of the experiment displayed in Fig. 2. The magnified core of the distribution in Fig. 3(d) corresponds roughly to Fig. 2(c). In the simulations, however, the statistics is better because of the larger number of grains in the cluster, so humps on the far tail can be observed in the zoomed-out image. These humps cannot be observed in Fig. 2(c) due to limited statistics. They do appear, however at later times in the experiments, as shown in Fig. 2(c), when the width of the distribution exceeds . This figure has not been reproduced in the simulations so far, because the simulations would have to run considerably longer.

We have also analyzed the displacement PDFs for a sub-ensemble of particles in the core of the hard-wall cluster (see Fig. 1(d)). These particles are completely trapped in their potential wells in the lattice. It turns out that in such a purely crystalline state the displacement PDFs on all time scales are Gaussian.

Now let us discussed simulations performed for parabolic potential confinement. As discussed above, to simulate quasi-2D the motion in the vertical component is severely restricted. That results in the behavior of -component of displacements similar to the hard-wall confinement case, as seen from Fig. 4. The PDFs of horizontal displacements, shown in Fig. 5, however still exhibit humps though much less pronounced because of the weaker confinement on plane. As shown in Fig. 5(d) it approaches an overall Gaussian shape on longer time scales.

Figure 4: (Color online) Langevin dynamics simulation of Yukawa system for the parabolic confinement case (stiff cluster). PDFs of vertical -component of displacements (dots) in units of , plotted for different time lags as indicated in the upper right corner. The full curve in (a) is a Gaussian with the same standard deviation.

In simulations of even softer states, though still with preservation of the regular lattice structure on the smallest time scales, stretched Gaussian distributions still appear on the time scales for which the standard deviation of the displacements is less than , but on longer time scales the PDF tends to develop humps on spatial scales much larger than (Fig. 6 (d)). Such features were also observed in the soft experiment (see PRL (), Fig. 4(a)), and was attributed to the formation of vortical flows on spatial scales extending from up to the cluster size.

This soft state has also been run in a pure 2D configuration, i.e. without -component, with results similar to those presented in Fig. 6. A preliminary fully 3D simulation of this state also yields qualitatively similar results, and this indicates that dimensionality is not a critical issue. The qualitative features described here are robust and universal for Langevin dynamics of Yukawa clusters with partial preservation of crystalline order. These studies will be published in a forthcoming paper.

Moreover, in these softer states, the system self-organizes into vortexes, or if stiffer, into rotating hexagonal domains which continuously break up and merge. The effect, called “cooperative hopping”, was first reported in 2D dusty plasma clusters in LinI2002 (). Large-scale vortexes driven by stochastic forcing have been observed experimentally PRL () and reproduced by the code used in the present study in Ref. NPJ (). By plotting the particle positions and their pre-history over a suitable short time-interval can give an impression of the velocity-field of the vortical flow. If this is done in successive time frames one can construct movies of this velocity field, which are very instructive to watch. Such movies for examples of experimental and simulated flows can be found as auxiliary material to Ref. NPJ (). In Refs. PoP (); PRL () one can find triangulation diagrams showing the occurrence of 5-fold and 7-fold defects associated with this hopping.

Figure 5: (Color online) Same as in Fig. 4, but now for the horizontal displacements .
Figure 6: (Color online) Same as in Fig. 5, but now for the soft cluster.

Iv Memory effects and intermittency

Information about the memory effects in the transport characteristics can be obtained from the variogram of particle displacements defined as

(5)

where we have introduced the position increments over the time lag . For a fractional Brownian motion (fBm) the PDF of is Gaussian, and , where is the Hurst exponent. Normal diffusion corresponds to Gaussian PDF and (Brownian motion). different from 0.5 is usually referred to as sub- or superdiffusion, and indicates violation of the central limit theorem, which implies that either the displacements are not identical and independent random variables and/or each of them has a heavy-tailed distribution with infinite variance. The latter is not the case in our experiments and simulations. The limit corresponds to ballistic motion.

In interpreting displacement variograms one has to realize that large-scale motions also influence the variogram on short time scales, so the Hurst exponent obtained on short-time scales does not necessarily reflect the nature of the diffusion of a particle relative to its nearest neighbors. Consider, for instance the extreme case of a frozen “flake” of dust grains which are completely fixed relative to each other, but that the flake itself is subject to transport characterized by a certain Hurst exponent. Then the variogram of every particle in the flake is characterized by this exponent, while their relative diffusion is negligible. In order to study this relative diffusion we would have to consider the evolution of relative position between neighboring particles.

Information about can also be obtained from the power spectral density of the particle displacement as a function of time. A power-law form of the spectrum, , corresponds to an fBm with . Thus normal diffusion requires .

The main departure from Gaussianity observed in our displacement PDFs is a flatter (more heavy-tailed) appearance, often well presented as a stretched Gaussian. A convenient measure of the flatness is the the kurtosis, which is the ratio between the fourth moment and the squared variance of the distribution. For the Gaussian the kurtosis is 3, and is higher for more heavy-tailed distributions. In the theory of turbulence, the concept of intermittency is used for situations where the PDFs have higher kurtosis on small than on large scales Frisch (). In our context intermittency would require that the kurtosis of displacement PDFs decreases with increasing time scale.

iv.1 Laboratory results

For the laboratory data of the stiff cluster, the power spectral density, autocorrelation function and variogram of particle displacements are presented in Figs.  3(a,b) of Ref. PoP (). In this experiment the PDF is non-Gaussian and self-similar on the short time scales, and the transport is superdiffusive with Hurst exponent (Fig. 6(a) of Ref. PoP ()). From results presented here, Fig. 2, it is apparent that on scales the displacement PDF approaches a Gaussian, so the kurtosis declines towards 3 at longer time scales. This indicates some intermittency - the displacements are more bursty on small scales than on large scales.

For the softer cluster, the power spectra are presented in Figs. 4(c,d) of Ref. PRL () and the variogram in Fig. 3(b). The transport is superdiffusive with on time scale and with for . By watching the movies of the particle motion one cannot avoid noticing that a common mode of motion the “minimal vortex” consisting of a stationary dust grain about which its six nearest neighbors rotate. This constitutes a nearly ballistic motion on the time scale , and might be the main contribution to the high value of observed on scales . On longer time scales vortex motions on increasing scales are responsible for this memory-based superdiffusion. On the time scales one could follow the displacements in this experiment the PDF develops some large humps due to long-lived, large vortices, and the tails are cut off by the finite size of the cluster. Hence, this experiment cannot tell us about the fate of the PDF on very large scale in extended systems.

Figure 7: (Color online) Variograms in units of , where is defined in Eq. (5) (top panel (a)). (): Boundary region of hard-wall potential, corresponding to PDFs in Fig. 3. (): Parabolic confinement the case of stiff cluster, corresponding to PDFs in Fig. 5. (): Parabolic confinement, the case of soft cluster, corresponding to PDFs in Fig. 6. Kurtosis as function of (lower panel (b)). The symbols represent the same states as in panel (a).
Figure 8: (Color online) Displacement autocorrelation function (ACF) for the hard wall confinement case. The symbols represent the same state as in Fig. 7 (a). The sampling interval used is 0.01 .

In the experiments on cold dusty-plasma liquids reported in Ref. LinI2002 () superdiffusive transport with is found for , and normal diffusion () on larger scales.

iv.2 Langevin dynamics simulation results

Variograms for different runs with varying stiffness are presented in Fig. 7(a). The variogram for the stiff core of hard-wall confinement is flat after a certain time (), and on average particles do not travel more than , and is not plotted in the figure.

The curve represented by the - symbols is representative for particles from the looser boundary regions of hard-wall potential runs. Such particles are able to escape caging, but the transport is subdiffusive () even for long time scales. The curve has an “S-shape” typical for cases when an oscillatory component is present in the time-series. The same should be reflected in autocorrelation function of the signal. Indeed, in Fig. 8 we find a clear periodicity on the relevant time scale.

For simulations of stiffer states with parabolic potential (the curve represented by () - symbols) the caging of particles is still noticeable for but for large times the Hurst exponent is higher, .

For simulations of soft states with parabolic potential the variogram (the curve with () - symbols the effect of caging is less prominent, but in the limit of large we find also find for this case.

The general picture for all states simulated (except when caging is total) is that for the PDFs are stretched Gaussians (with humps superposed for the stiffer states), and the diffusion is slightly subdiffusive - more so for the stiffer states. These distributions exhibit heavier tails than Gaussians, and hence kurtosis (flatness) higher than 3. For the PDFs seem to tend more towards Gaussian again, at least when they are smoothed to remove the humps. This can be seen by plotting the kurtosis against the standard deviation as done in Fig. 7(b). It is observed that in general the flatness increases with time as long as the standard deviation , but have a clear descending trend towards the Gaussian value (3) as exceeds . For completely caged particles the kurtosis remains close to 3, confirming that the PDF remains Gaussian for these particles.

The concept of intermittency in a signal is loosely defined as the tendency of a signal to be more bursty on short scales than on long scales Frisch (). This implies higher kurtosis on small than on large time scales. In our study this is the case on the “hydrodynamic” scales, , but not on the scales of caging, .

V The origin of non-Gaussian displacements

The Langevin thermostat used here models the interaction of the Yukawa many-body system with a heat bath of temperature , and hence represents a canonical statistical ensemble. Thus the simulated system should relax to a thermodynamic equilibrium. With proper tuning of control parameters our system develops strong fluctuations, which in NPJ () was shown to exhibit (imperfect) scaling. This makes it natural to think about this as equilibrium critical behavior. Since this behavior is observed only when the control parameters are in a range where the system is subject to some local positional order, we believe it is associated with a continuous solid-liquid phase transition. However, the small size and strong inhomogeneity of the systems simulated excludes direct comparison with theory review () and earlier simulations Hartmann () for such transistions in 2D Yukawa systems.

In extensive systems [(systems without long-range interactions)], thermodynamic equilibrium implies Gibbs-distributed microstates of the cluster. This, however, does not exclude non-Gaussian distribution of particle displacements on varying time scales. In order to obtain some insight into the origin of this non-Gaussianity it may be useful to write a Langevin equation for a single dust grain in the form:

(6)
(7)

where is the self-consistent (time-averaged) caging potential well that a partially caged dust grain experiences, is the additional fluctuating (stochastic) force field due to the Yukawa forces from the motion of the neighboring dust grains, is the dust-neutral collision frequency, represents the diffusion coefficient due the stochastic force arising from collisions with neutrals, and is the vector of three independent Wiener processes (Brownian motions).

Let us first recall some results on free diffusion of a dust grain imbedded in a neutral gas, i.e. let us neglect the term in square brackets on the right hand side of Eq. (7). For a particle starting at rest at the origin at time , the equations can be integrated to yield Gardiner () , for . On time scales the collision term is unimportant, and the velocity is a Wiener process. On these time scales the position process is the integral of the Wiener process, and is ballistic. The variogram would yield . For the velocity increments will be independent and Gaussian (white noise), and the position increments (displacements) will be Gaussian and a Brownian motion, i.e. the slope is in the variogram.

If we introduce a stationary potential structure, but still neglect the stochastic force due to grain-grain collisions, there is a well-defined Fokker-Planck equation formulated in 6-dimensional phase space associated with Eq. (7), which features the Gibbs distribution as a stationary solution, and in configuration space we have the Boltzmann-distribution .

If the caging potential barriers are much higher than the thermal energy of the grains, the cluster is in a completely frozen crystalline state, there is no diffusive transport beyond the mean interparticle distance.

The omission of the stochastic force due to grain-grain collisions is only valid on time scales , where is essentially the time it takes for a grain to bounce off the walls in its cage. The typical situation in our experiments and simulations is that . On time scales , as explained above, the motion is ballistic. If the velocities are Maxwellian due to the Langevin thermostat, the displacements will be Gaussian distributed for . This is what we observe in the simulations. In the experiments discussed in this paper we observe non-Gaussian displacements already for , but this is because the sampling time in the experiment is somewhat longer than the grain-grain collision time. This is supported by the results reported in Knapek (), where Gaussian displacements were found for in an experiment where particle positions were sampled at 500 Hz.

On time scales a single-particle stochastic equation makes sense only if the force due to grain-grain interaction is represented as a stochastic source term. If the issue under consideration is grain transport, the stochastic equation can be simplified by averaging the equations over a time scale of the order , and obtain an equation for the averaged position. This justifies to neglect the inertial term in Eq. (7) (the Smoluchowski approximation), which then reduces to the

(8)

where represents the stochastic force due to collisions with neutrals as well as other dust grains. A problem is of course that the interaction contains long-range spatiotemporal dependencies and the statistical distribution of momentum transfers may be non-Gaussian, and hence cannot reliably be represented by a white noise term. One could certainly make assumptions about the statistical nature of the interaction, but the standard derivations of the associated Fokker-Planck equation are no longer valid since the position is no longer a Markov process.

Another approach would be to assume that the time-averaged potential is constant in the interior of the cluster, and to incorporate the the effects of the dust-dust interaction in the friction term and the stochastic term in Eq. (7). The resulting stochastic equation would take the form (for simplicity we write the one-dimensional version):

(9)

where the drift term represents a generalized friction due to combined action of the dust-dust collisions and the dust-neutral collisions, and the second term on the right represents the stochastic part of these interactions. In the following we shall assume that the latter contains no long-range memory and can be represented as Gaussian white noise. An equation of this form was studied by Kaniadakis and Quaraty Kaniadakis (), and by Borland Borland () in the context of determining the conditions and must satisfy for the resulting stationary velocity PDF to reduce to the Tsallis distributionTsallis1 (). If the stochastic equation is interpreted in the sense of Itô (see for instance Gardiner ()), the associated Fokker-Planck equation for the velocity distribution is

(10)

If the drift term has a form that confines the particles to a range with finite velocities (which will be the case for a physically meaningful friction term) the stationary solution to Eq. (10) can be written as

(11)

where is a normalization constant. In the case of linear friction and constant diffusion coefficient Eqs. (9) and (10) represents the well-known Ornstein-Uhlenbeck problem, and the solution (11) is the resulting Maxwell velocity distribution. Borland Borland () shows that a general criterion for the solution (11) to reduce to the Tsallis distribution Tsallis1 ()

(12)

is that satisfy the relation

(13)

Here is the inverse temperature and is the non-extensivity parameter. For the distribution reduces to the Maxwellian, and the family of functions that gives this conventional extensive Gibbs-Boltzmann statistics is given by the relation

(14)

For constant diffusion coefficient this reduces to , where satisfies the relation , which is a version of the fluctuation-dissipation theorem.

Borland emphasizes that Eq. (13) implies that there is a whole family of functions which give rise to Tsallis statistics, but it should maybe also be mentioned that there exists an infinitely larger family of functions that do not. Thus, the ubiquity of Tsallis statistics in this context relies on the existence of ubiquitous physical situations where Eq. (13) is fulfilled. The analysis of our experiments and simulations shows that the displacement PDFs are well described by stretched Gaussians with on time scales in the range , and by Gaussians in the range . In Fig. 9 we demonstrate that the stretched Gaussian with is practically indistinguishable from the Tsallis distribution with , so there is no information in the experimental data to prefer one to the other. On the other hand the stretched Gaussian provides a very simple and physically interpretable generalization of the Ornstein-Uhlenbeck problem, as will be described in the following.

Figure 9: (Color online) The red curve is a log-plot of the stretched-Gaussian function vs. for and . The blue curve is a corresponding plot of the Tsallis distribution for . The values for and are typical for the experimental results discussed in this paper.

Let us consider the Itô-Langevin equation Eq. (9) with constant diffusion coefficient , and generalized friction term

(15)

The physical rationale for such a sub-linear friction term is simply to account for the reduced effective dust-dust friction introduced by those fast particles undergoing cooperative hopping. It has been shown Reichardt2003 (); Zangi () that this hopping takes place along string-like structures of defects, and hence it is more natural to model it as a modification of the directed friction force than as modification of the diffusion coefficient.

In Eq. 15 the case corresponds to the standard Ornstein-Uhlenbeck problem, and would correspond to a friction that grows as the square root of the velocity, rather than proportional to the velocity. The stationary solution to the associated Fokker-Planck equation given by Eq. (11) reduces to the stretched Gaussian

(16)

At this point we should keep in mind that the stretched Gaussian Eq. (4) found in our data are PDFs for the position displacements at varying time lags , not the velocity PDFs. In order to find the displacement PDFs we have integrated numerically the stochastic equation (9) with the generalized friction term (and ) for an ensemble of initial velocites drawn from the stretched-exponential distribution Eq. (16). Then we have found the position trajectories by integrating , and formed the displacement PDFs for different time lags. The rather obvious result is that the displacement PDF remains close to the stretched Gaussian for and converges to a Gaussian for . The reason for this is that the displacements are near ballistic for , and hence reflect the velocity distribution. On time scales greater than the velocity process is de-correlated and stationary, and successive displacements can be considered as independent, identical random variables. Displacements , for , can therefore be considered as a sum of identical, independent random variables, and thus the conditions of the central-limit theorem are satisfied. Thus the displacement PDF should be Gaussian and the diffusion should be normal (Brownian motion). The variograms produced on the basis of the computed PDFs shows (obviously) that for and for , but also that there is a large transitional regime of time scales where the slope corresponds to Hurst exponents in the range .

This extremely simplified stochastic model reproduces the stretched exponentials observed for , and the convergence to Gaussian for observed in our simulations. Since the sampling time in the simulations are of the order of the variograms in Fig. 7 do not show the ballistic regime where , but the behavior of the variograms in the regime can be interpreted as a slow convergence towards a Brownian motion (). It is also noteworthy that the simulations in Zangi (); Reichardt2007 () gave rise to similar variograms when the system was in the hexatic phase between a solid and a liquid. Those simulations were performed with periodic boundary conditions, so the effects of the finite systems size and the system inhomogeneity did not influence the variogram at large times as they do in our simulations. Since the simulation in Zangi () also displays a leptokurtic distribution on the scales , and a transition to a Gaussian for , we conclude that the stochastic model, and the associated Fokker-Planck equation, yields a reasonable lowest-order description of anomalous diffusion in 2D many-body systems in the hexatic phase.

The linear Fokker-Planck approach discussed above (including the cases discussed by Borland) implies Gaussian displacement distribution in the limit . Hence it cannot be used to describe anomalous diffusion in the long-time limit. Another formulation that allows non-Gaussian displacement distributions and anomalous transport is the nonlinear Fokker-Planck equation Plastino (); Tsallis2 (); Borland2 (),

(17)

In order to describe anomalous displacement diffusion should now be interpreted as a spatial variable, and we should focus on time-dependent solutions. For this particular nonlinear diffusion term, and a linearly varying drift term , such a time-dependent solution takes the form of a Tsallis distribution, Eq. (12), where and now are time dependent. In the case of free diffusion , the variance of the distribution has the time-asymptotic dependence

(18)

provided . For the distribution has a power-law tail , and for the tail is so heavy that the variance does not exist. For we have power-law tail and , implying superdiffusion. For the distribution reduces to a Gaussian and we have normal diffusion, and for the Tsallis distribution has a cut-off in the tail ( for ), and the transport is subdiffusive. Thus the Tsallis relation (18) implies that distributions with tails heavier than the Gaussian (leptokurtic) must be associated with superdiffusion. Our simulations are subdiffusive for , but the PDFs are leptokurtic and well described by the Tsallis distribution with , which according to Eq. (18) should give a weakly superdiffusive transport. This inconsistency indicates that the nonlinear Fokker-Planck equation is not a good description of the transport observed in our simulations.

There are also considerable difficulties associated with the physical interpretation of Eq. (17) for our case. Borland Borland2 () attempts to provide such an interpretation by considering as a -dependent diffusion coefficient, that could replace in the stochastic equation (9) (since we are considering spatial diffusion, the variable in that equation should now be interpreted as a spatial variable, so we are really dealing with the Smoluchowski equation (8)). If could be interpreted as a density, there would be no problem to envisage a density-dependent diffusion coefficient, but the density of dust grains in our system is almost constant in space and time, so a spatial diffusion equation for density does not make sense. will have to be interpreted as a probablity density for an ensemble of independent particle trajectories starting out at positions selected from a prescribed initial distribution in different independent realizations of the experiment. Since we are interested in the evolution of particle displacements a natural choice is to consider an ensemble of particles starting from the same postition , i.e. . The quantity obviously depends on the choice of initial postion , and therefore cannot be a local physical property of the medium at the point at . It is rather a quantity that is valid only for the particles belonging to this specific ensemble (i.e. the particles starting out at the position at ), and hence such a model would imply that the diffusion properties of a particle depend very strongly on its prehistory, i.e. there must be strong long-range memory in the system.

Vi Conclusions

In this paper we have studied anomalous transport properties; non-Gaussian particle displacement statistics and memory effects, in a Langevin-dynamics model, and we have contrasted these simulations with experimental results from quasi-2D dust plasma clusters in soft states. We have demonstrated that anomalous transport is ubiquitous on time scales provided the system is not residing in the pure crystalline or liquid phases. Moreover, we have shown that this complex dynamics emerges from stochastic forcing and dissipation provided by the collisions with the neutral gas, and that no other plasma effects than the static Debye screening are required.

From the experiments and the Langevin dynamics simulations we observe that Gaussian displacement distributions are restricted to the following cases: (i) on time scales less than the collision time in all systems, (ii) on all time scales for systems that are so stiff that no hopping takes place (pure crystal), (iii) on all time scales for systems where no caging occurs (pure liquid or gas), (iiii) for time scales longer than in soft systems.

A result that seems to be robust for both stiff and soft states, is that PDFs evolve from a leptokurtic (heavy-tailed) shape for small time-lags towards a Gaussian shape for larger . This feature is usually interpreted as a signature of intermittency - a spikyness in the flow-field which gives rise to more leptokurtic PDFs of the displacements on the small scales. Note that intermittency does not prevail to spatial scales less than . A simple way to model this intermittency feature is via the single-partice stochastic equation (9), and the associated linear Fokker-Planck equation (10), with a non-linear drift term given by Eq. (15).

In Ref.  PRL () it is pointed out that the dust monolayer should be perceived as a viscoelastic medium, where the elastic properties dominate on the smaller scales. Thus the transition from stretched-Gaussian to Gaussian PDFs could correspond to the transition from elastic to viscous flow. One future goal would be to perform experiments and simulations on sufficiently large spatial and temporal scales to characterize the transport associated with homogeneous, turbulent flow in such systems. With such extensive simulations one could clarify, for instance, if energy will cascade to vortices on infinitely large scales in an infinite system, or if there is an upper limit to the vortex size related to the characteristic length over which elasticity dominates over viscosity.

The rather imprecise qualifier “soft” has been employed in this paper to characterize 2D dusty plasma clusters which preserve local hexagonal order, but exhibit loss of such order on larger scales. Materials displaying such properties are also classified as “hexatic”, and the continuous transition from the crystalline to the liquid state might be considered as a continuous phase transition Christensen (). In NPJ () we perform a particular avalanche analysis of the experimental soft cluster and a Langevin-dymamics simulation. In this analysis we define connected space-time regions where the kinetic energy of the grains exceeds a prescribed threshold, and define the activity in these regions as avalanches. The statistics of avalanche sizes and durations tend to obey power laws with similar characteristic exponents for experiment and simulation, which are properties characteristic for critical phenomena and higher order phase transitions Christensen (). Such phenomena have been studied in strongly idealized models such as the Ising model Christensen (); Gitterman () and the XY model Gitterman (), but the Yukawa-Langevin model studied in this paper exhibits, in spite of its simplicity with respect to the physical interactions, the prospect of quantitative prediction of dynamics in real physical systems where the microscopic state of the system can be tracked to the smallest detail of physical interest.

Acknowledgements.
S.R. acknowledges support of the Swedish Research Council. K. R. acknowledges support of the Norwegian Research Council under grant 171076/V30, and is grateful to Dr. Martin Rypdal for helpful discussions and for providing numerical solutions to Eq. (9). The authors also acknowledge several helpful comments from anonymous referees.

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