# Emergence of collective motion in a model of interacting Brownian particles

###### Abstract

By studying a system of Brownian particles, interacting only through a local social-like force (velocity alignment), we show that self-propulsion is not a necessary feature for the flocking transition to take place as long as underdamped particle dynamics can be guaranteed. Moreover, the system transits from stationary phases close to thermal equilibrium, with no net flux of particles, to far-from-equilibrium ones exhibiting collective motion, long-range order and giant number fluctuations, features typically associated to ordered phases of models where self-propulsion is considered.

###### pacs:

87.10.-e, 05.70.Fh, 05.40.-a, 05.70.Ln^{†}

^{†}thanks: author to whom correspondence should be addressed.

Collective motion is an ubiquitous phenomenon in biological groups such as flocks of birds, schools of fishes, swarms of insects, etc. The study of these far-from-equilibrium systems has attracted great interest over the last few decades, as the spontaneous emergence of such ordered phases and coordinated behavior, arising from local interactions, cannot be accounted for by the standard theorems of statistical mechanics vic12 ().

Introduced almost twenty years ago, the seminal model by Vicsek et al. vic95 () provided a simple tool to study the transition to collective motion, in a non-equilibrium situation, taking into account two basic ingredients: the self-propulsive character of the particles and a local velocity-alignment interaction among them. Due to the discrete nature of the model, a given particle instantaneously orients its direction of motion along the average direction of motion of its neighbors within a radius , while stochastic perturbations are considered by adding a random angle (“noise”) to this direction. In two dimensions, the system displays an ordered phase characterized by collective motion with long-range order and giant number fluctuations ton05 (), just below a critical value of the noise intensity that depends on the particle density. It is in this respect that this model can be considered as a paradigm of non-equilibrium phase transitions, since such ordered phases are forbidden in equilibrium (for Heisenberg-like models) by the Mermin-Wagner-Hohenberg theorem mer66 (). Above this value, the ordered phase breaks down into a stationary, disordered and out-of-equilibrium one.

Over the years, many generalizations of the model have been developed, keeping self-propulsion as an essential ingredient for the phase transition to take place, in combination with interactions of the “social” type among the particles such as velocity-alignment gre04 (); gin10 (). This has led to the development of sophisticated nonlinear friction terms erd02 (); dos09 (), a bias that may be justified arguing, on the one hand, that the concept of self-propelled (or active Brownian) particles captures the natural ability (seen in many biological systems) for the agents to develop motion by themselves sch07 (); gro12 () and, on the other, that it is an important ingredient for pattern formation in models of collective motion shi96 ().

In this Letter, we study the emergence of collective motion in a two-dimensional system of passive Brownian (not-self-propelled) particles that interact among themselves only through local forces of the social type (velocity-alignment in this case). In such a way, we show that the symmetry breaking of the disordered phase corresponds to the breakdown of a close-to-equilibrium state for a particular value of the ratio between two characteristic time-scales in the system: one related to the mean collision time of Brownian particles immersed in a thermal bath, and the other related to the rate of alignment among particles. Our results show that local alignment interactions suffice for the development of collective motion, with true long-range order, whenever underdamped particles (for which inertial motion cannot be neglected) are considered. Through standard numerical measurements, the far-from-equilibrium nature of these states is stablished, as they exhibit typical features of this kind of phases such as giant number fluctuations among others.

Our model is described in terms of generic stochastic differential equations for Brownian particles restricted to move within a box of linear size with periodic boundary conditions, i.e.,

(1) |

where and is the mass of the particles. The last two terms on the right hand side correspond to the linear-dissipative and fluctuating forces that appear in the Langevin description of Brownian motion, respectively. The components of the vector are uncorrelated Gaussian white noises with zero mean and, because of the fluctuation-dissipation relation (FDR), with autocorrelation function , where is the -th Cartesian component of , is the Boltzmann constant, the temperature of the bath, and and are the Kronecker delta and the Dirac delta function, respectively.

The alignment behavior is implemented through the force , that corresponds to the two-dimensional form of , with being the unitary vector in the direction of and , while corresponds to the local instantaneous direction of motion, i.e., the arithmetic average of the direction of motion of the particles that surround the -th particle within a neighborhood of radius . The coupling factor is a measure of how fast the velocity vector of a single particle aligns along the direction of . It is easy to check its non-propelling character since . The alignment interaction considered here corresponds to a simple generalization, with a finite aligning rate, of the one introduced in vic95 (). We must mention that alignment interactions with finite aligning rates have been considered before in some other forms dos09 (); gro12 (); mog96 ().

We choose as time, speed and length scales the quantities: , and , respectively. In this way, the number of independent parameters in our model is reduced to three: the dimensionless alignment-coupling constant , the dimensionless interaction range , and the dimensionless particle density with . Without loss of generality, we fix further on. All numerical results presented here, were obtained by integrating the set of Eqs. (1) with a modified version of the velocity-Verlet algorithm gro97 () with an integration time-step . Random initial conditions where taken for the position of the particles while their initial velocities where drawn from the equilibrium Maxwell-Boltzmann velocity distribution.

In the absence of interactions (), the particle dynamics is constrained by the FDR as in the standard description of Brownian motion, therefore, the stationary-state distribution of the single particle velocities corresponds to that of equilibrium with the highest rotational symmetry. Interestingly, for small values of , where the alignment time-scale is smaller than that related to the FDR, the system remains in a disordered phase still characterized by properties of thermal equilibrium with no net transport, normal diffusion of individual particles and Maxwellian probability densities of single particle velocities as shown in Fig. 1(a).

As increases above a critical value, the system develops a self-induced far-from-equilibrium phase that exhibits a net flux of particles and non-Maxwellian probability densities of single particle velocities as shown in Fig. 1(b). We characterize the ordered collective motion in this phase through the accumulated order parameter , that is calculated from the instantaneous with defined from . The critical point that separates the disordered and ordered phases decreases with , reaching a limit value when , that corresponds to that of the globally-coupled (GC) regime () [Fig. 2(a)]. This ordered phase exhibits typical features of far-from-equilibrium ordered phases present in models that consider self-propulsion. For instance, our model shows giant number fluctuations, that is a signature of fluctuating ordered active phases ton05 (), here characterized by , corresponding to the square root of the variance of the particles contained ( in average) in square boxes of linear size . For our model, scales like with [Fig. 2(b)]. This value is, however, larger than that known for the Vicsek et al. model and its generalizations gin10 ().

Surprisingly, even with self-propulsion left aside, our model exhibits true long-range order as shown in Fig. 2(c), where the order parameter slowly decays (algebraically) with to a constant value for all of the particle-density values considered here. Moreover, dilute systems with, e.g., , show what seems to be intermittent behavior (also present in the original Vicsek et al. model hue04 ()), where displays an asymmetric Gaussian form with an exponential tail as shown in Fig. 2(e). Segregation decreases with , while the distribution of approaches a Gaussian one, with showing less spikes of instantaneous disorder as a function of [Figs. 2(d) and 2(e)]. This is due to the fact that, as increases, the particles in the system become more homogeneously distributed over space [Fig. 3]. In fact, as or if global coupling () is considered, this feature allows for the analytical treatment of the model where the instability of the disordered close-to-equilibrium state can be demonstrated, and the relation of our model to the Kuramoto model of synchronization is revealed. This case is discussed in details in sev14 ().

Another feature displayed by ordered far-from-equilibrium phases, whenever the interactions depend on the distance, is the strong coupling between local density and local order gre04 (); gin10 (). As shown in Fig. 3 for our model, this feature is more evident for dilute more-segregated systems, as the particles tend to concentrate in a few very dense and very ordered clusters. This behavior also decreases with , due to the fact that the system becomes more homogeneous and correlated. See, for example, that the snapshots for the direction field (right column of the figure) show less white spots as increases, meaning that, wherever there is color, there are at least a few particles with their mean direction in correspondence to the color key.

Results regarding the nature of the disorder-order phase transition displayed by our model are presented in Fig. 4. On the left column, the distribution shows a single-peaked form around for the systems considered here. Additionally, on the right column, the behavior of the Binder cumulant vs , for different system sizes, shows a smooth behavior without any signs of discontinuity. Even more, there are no signs of the emergence of density waves, present in some models that consider self-propulsion and display a discontinuous phase transition gre04 (). All of these facts hint the continuous character of the phase transition in our model.

It is interesting to notice, though, that the phase transition of our model takes place for finite values of even in the limit cases when or when global coupling is considered sev14 (). In contrast, in the Vicsek et al. model and some of its generalizations, in the same limits, the disordered phase only occurs at maximum noise (or, equivalently, in the infinite temperature limit) dos09 ().

We must mention that, due to the stronger fluctuations of for dilute systems, the computing time required is larger than that required for systems with higher particle density, nonetheless, denser systems include more particles than dilute ones for the same values of . For instance, our runs for the largest dilute systems required about integration steps. Even so, longer integration times with larger systems are required for the determination of quantities such as critical points and exponents for the different cases considered here. Moreover, larger systems require longer integration times due to the locality of the interactions. These calculations are beyond the computational resources available to us at the moment, however, we are woking on to study this in the future.

In summary, our results show that non-Hamiltonian interactions that do not preserve momentum (such as the alignment interaction typically used to model flocking behavior), in combination with underdamped particle dynamics, are able to drive the system from an close-to-equilibrium (disordered) phase to a far-from-equilibrium (ordered) one in a novel type of phase transition. Thus, we believe our model is suitable for studying the passage from states where the entropy is maximized to stationary phases where entropy is produced. We are currently pursuing this line of investigation. In addition, under such circumstances, we have also demonstrated that self-propulsion is an unnecessary feature for systems to develop long-range order out of local interactions, even in two dimensions, as typically considered by some other models for flocking.

Beyond the obvious implications in the study of flocking phenomena, we believe our results are relevant in the more general context of the study of phase transitions in equilibrium or out-of-equilibrium statistical mechanics.

###### Acknowledgements.

The authors gratefully acknowledge the computing time granted on the supercomputers MIZTLI (DGTIC-UNAM), THUBAT-KAAL (CNS-IPICyT) and, through the project “Cosmología y astrofísica relativista: objetos compactos y materia obscura”, on XIUHCOATL (CINVESTAV). V.D. acknowledges support from the grant PROMEP/103.5/10/7296 and from CONACyT. F.J.S. acknowledges support from the grant PAPIIT-IN113114.## References

- (1) T. Vicsek and A. Zafeiris, Phys. Rep. 517, 71 (2012).
- (2) T. Vicsek, A. Czirók, E. Ben-Jacob, I. Cohen, and O. Shochet, Phys. Rev. Lett. 75, 1226 (1995).
- (3) J. Toner, Y. Tu, and S. Ramaswamy, Ann. Phys. (N.Y.) 318, 170 (2005).
- (4) N.D. Mermin and H Wagner, Phys. Rev. Lett. 17, 1133 (1966); P.C. Hohenberg, Phys. Rev. 158, 383 (1967); N.D. Mermin, J. Math. Phys. 8, 1061 (1967).
- (5) G. Grégoire and H. Chaté, Phys. Rev. Lett. 92, 025702 (2004); H. Chaté, F. Ginelli, G. Grégoire, and F. Raynaud, Phys. Rev. E 77, 046113 (2008).
- (6) F. Ginelli and H. Chaté, Phys. Rev. Lett. 105 168103 (2010).
- (7) U. Erdmann, W. Ebeling and V.S. Anishchenko, Phys. Rev. E 65, 061106 (2002); U. Erdmann, W. Ebeling and A.S. Mikhailov, Phys. Rev. E 71, 051904 (2005).
- (8) V. Dossetti, F.J. Sevilla and V.M. Kenkre, Phys. Rev. E 79, 051115 (2009).
- (9) F. Schweitzer, Brownian Agents and Active Particles: Collective Dynamics in the Natural and Social Sciences (Springer-Verlag, Berlin, 2007).
- (10) R. Grossmann, L. Schimansky-Geier and P. Romanczuk, New J. Phys. 14, 073033 (2012).
- (11) N. Shimoyama, K. Sugawara, T. Mizuguchi, Y. Hayakawa, and M. Sano, Phys. Rev. Lett. 76, 3870 (1996); W. Ebeling and U. Erdmann, Complexity 8 (4), 23-30 (2003); W. Ebeling and U. Erdmann, Complexity 8 (4), 23 (2003); J.R. Touma, A. Shreim, and L.I. Klushin, Phys. Rev. E 81, 066106 (2010).
- (12) A. Mogilner and L. Edelstein-Keshet, Physica D 89 346 (1996); C.R. McInnes, Phys. Rev. E 75, 032904 (2007); F.D.C. Farrell, M.C. Marchetti, D. Marenduzzo, and J. Tailleur, Phys. Rev. Lett. 108 248101 (2012).
- (13) R. D. Groot and P. B. Warren, J. Chem. Phys. 107, 4423 (1997).
- (14) C. Huepe and M. Aldana, Phys. Rev. Lett. 92, 168701 (2004).
- (15) J.A. Acebrón, L.L. Bonilla, C.J. Pérez-Vicente, F. Ritort, and R. Spigler, Rev. Mod. Phys. 77 (1), 137 (2005).
- (16) F.J. Sevilla, V. Dossetti, and A. Heiblum-Robles, arXiv:1408.3567