Impact Factor 2.638 | CiteScore 2.3
More on impact ›

Original Research ARTICLE

Front. Phys., 17 January 2014 |

Cyclic and coherent states in flocks with topological distance

  • 1Department of Theoretical Sciences, Satyendra Nath Bose National Centre for Basic Sciences, Kolkata, India
  • 2Department of Physics, Birla Institute of Technology and Science, Pilani, India

A simple model of the two dimensional collective motion of a group of mobile agents has been studied. Like birds, these agents travel in open free space where each of them interacts with the first n neighbors determined by the topological distance with a free boundary condition. Using the same prescription for interactions used in the Vicsek model with scalar noise it has been observed that the flock, in absence of the noise, arrives at a number of interesting stationary states. One of the two most prominent states is the “single sink state” where the entire flock travels along the same direction maintaining perfect cohesion and coherence. The other state is the “cyclic state” where every individual agent executes a uniform circular motion, and the correlation among the agents guarantees that the entire flock executes a pulsating dynamics i.e., expands and contracts periodically between a minimum and a maximum size of the flock. We have studied another limiting situation when refreshing rate of the interaction zone (IZ) is the fastest. In this case the entire flock gets fragmented into smaller clusters of different sizes. On introduction of scalar noise a crossover is observed when the agents cross over from a ballistic motion to a diffusive motion. Expectedly the crossover time is dependent on the strength of the noise η and diverges as η → 0. An even more simpler version of this model has been studied by suppressing the translational degrees of freedom of the agents but retaining their angular motion. Here agents are spins, placed at the sites of a square lattice with periodic boundary condition. Every spin interacts with its n = 2, 3, or 4 nearest neighbors. In the stationary state the entire spin pattern moves as a whole when interactions are anisotropic with n = 2 and 3; but it is completely frozen when the interaction is isotropic with n = 4. These spin configurations have vortex-antivortex pairs whose density increases as the noise η increases and follows an excellent finite-size scaling analysis.

1. Introduction

Flights of a flock of birds or a swarm of bees are well known examples of living systems exhibiting collective behavior which are often modeled by groups of self-propelled mobile agents [14]. These groups are called “cohesive” since each agent maintains a characteristic distance from other agents and at the same time they are “coherent” since all agents move along a common direction. In addition, the internal structure and organization of a flock is found to be complex and far from being static. Examples include leader-follower relationships in bird flocks [5], fission-fusion events in fish schools [6] and social groups in human crowd [7]. Such flocks often travel over long duration covering distances much larger than the size of the flocks along arbitrary directions and therefore effectively an infinite amount of space is available to the flock for it's motion. It is also known that while individual agents often change their directions of flight the whole flock maintains motion along the same direction in a stable fashion.

A generic feature of collective motion is, agents are short-sighted. While an individual agent's behavior is influenced by the behavior of a small group of local agents around it, the whole group behaves in unison. In other words, a short range interaction among the agents may lead to a unique global behavior of the entire group which implies the existence of a long range correlation among the agents. Therefore the question is, given a random distribution of positions and velocities what kind of short range dynamics can lead to global correlation reflected in cohesion and coherence among the agents.

This question was first explored in an assembly of self-propelled particles, known as the Vicsek model [8]. Here particles (agents) are released at random locations within a unit square box on the xy plane with periodic boundary condition and with random velocities. However, in the deterministic motion the direction of velocity of each agent i is oriented along the resultant velocity vRi of all agents within an interaction zone (IZ) of range R around i. In reality each agent may make an error in judging the resultant direction of motion and this has been introduced in the stochastic version of the model where noise is introduced by topping the orientational angle of vRi by a random amount Δθ. Each individual agent is then moved along the updated velocity direction. A coherent phase is observed in the noise-free case with high agent densities. Moreover a continuous phase transition is observed on increasing the strength of noise where the mean flock speed continuously decreases to zero. However, facets like high density traveling bands occurring at low noise were revealed in later studies [9, 10] and arguments were put in favor of a discontinuous transition.

In a recent field study by the Starflag group on flocks of Starlings [11], it has been shown that the interactions among the birds of a flock do not depend on the metric distance but on the topological distance. More quantitatively they found that each bird interacts with a fixed number of neighbors, about six or seven in number, rather than all neighbors within a fixed radial distance. Observing flocks of Starlings the angular density distribution of neighboring birds have been found to be anisotropic e.g., a bird is more likely to keep its nearest neighbor at its two sides rather than on the front and back. Fishes [12] have also been found to interact with neighbors determined by topological rules. Theoretical investigations [13, 14] revealed that the behavior of topology based models are very different from metric based models [15].

The concept of graph theory based topology was, however, used [16] to analyze the Vicsek model itself from the perspective of control theory. The metric distance based interactions were modeled using graphs with “switching topology.” Such studies also derived the conditions for the formation of coherent flocks for agents with fixed topologies [17]. The relevance of underlying graphs or networks on the nature of collective motion has also been studied [18, 19].

The observations of the StarFlag group prompted us to study the collective motion of flocking phenomena in two dimensions using the interactions depending on the topological distance. Most crucially we have obtained very interesting stationary states which have not been observed before, mainly the cyclic states (CS). At the same time an increasingly large number of states are found to be completely cohesive and coherent. The paper is organized as follows. In section 2 we describe our topological distance dependent model for collective motion. The connectivity among such a collection of agents has been studied as Random Geometric Graph (RGG) in section 3. The stationary states of such flocks have been studied in section 4, the two most prominent states being the Single Sink State and the Cyclic State. The effect of the noise on the dynamics and the critical point of transition have been studied in section 5. Study of the dynamics of the flock with the fastest refreshing rate of the IZ has been done in section 6. A simpler version of the model with its vortex-antivortex states have been studied on the square lattice in section 7. Finally we summarize and discuss our results in section 8.

2. Model

In our model the IZ has been defined in the following way. During the flight, each agent i interacts with a short list of n other selected agents that constitute the IZ. It determines it's own velocity using the Equation (1) given below following a synchronous dynamics. In general, the agent often refreshes the group of agents in IZ. For example, at the early stage, when the flock is relaxing to arrive at the stationary state and also during some stationary states, the inter-agent distances change with time. Every time the IZ is refreshed, we assume the criterion of selecting n agents is that they are the first n nearest neighbors of i. We introduce at this point a “refreshing rate” which controls how frequently an agent updates it's IZ. In this paper, we study two limiting situations when these rates are slowest and fastest. In the slowest rate, the agents do not change at all the list of other n agents in their IZs. The IZ for each agent, constructed at the initial stage, remains the same ever after, even if n initial neighbors of an agent no longer remain nearest neighbors as time proceeds. The other limiting case is when the refreshing rate is the fastest, the IZ is refreshed for every agent at each time step. The slowest case has been discussed in sections 4 and 5. The fastest refreshing rates have been discussed in section 6. For the spins on the square lattice discussed in section 7, these two cases actually mean the same since the spins are firmly fixed at their lattice positions.

The number n of agents in IZ is considered as an integer parameter of the model. As in Vicsek model [8] the system is updated using a discrete time dynamics. While the speeds v of all agents are always maintained to be the same, the orientational angles θi of their velocities are updated by the direction of the resultant of velocity vectors of all n agents in the IZ and the agent i itself (Figure 1),

θi(t+1)=tan1[Σjsinθj(t)/Σjcosθj(t) ](1)

where the summation index j runs over all (n + 1) agents in IZ. The whole flock moves in the infinite space. Following this dynamics, the flock reaches the stationary state after a certain period of relaxation time. It is observed that the stationary state depends on the initial positions, initial velocities of the agents, as well as the neighbor number n. Though a number of different stationary states have been observed, often the state is a fixed point or a cycle. We have studied the statistical properties of these fixed points and cycles and observed that cohesion and/or coherence are indeed present in different stationary states.


Figure 1. (A) A flock of N = 16 agents with n = 5 neighbors in the interaction zone and at any arbitrary time t. The central agent is denoted by the subscript 0 and the velocity vectors of this agent and its five neighbors in the interaction zone are shown using red arrows. (B) In the next time step the velocity of agent 0 is calculated by Equation (1) which is along the resultant of all n + 1 velocity vectors and has the magnitude v.

There are two crucial differences of our model and the Vicsek's model which we summarize as follows: (a) We have used the same prescription of interaction that had been claimed in the StarFlag experiment. Accordingly, an agent here interacts with a fixed number n of nearest neighbors and not with all neighbors up to a fixed radial distance. It may be noted that, these two mechanisms are essentially serving the same purpose. Both prescriptions keep the mutual interactions active among the local agents only. Therefore our choice of neighborhood and Vicsek model's range of interaction are actually on the same footing. (b) No periodic boundary condition is imposed in our model. Therefore agents move out in open space, yet they often form flocks that exhibit considerable amount of cohesion and coherence. Compared to the Vicsek model, use of the free boundary condition makes our model less restrictive.

In the limiting case, when the IZ is refreshed at the slowest rate, it may appear that for an agent, any of the n neighbors can be at an arbitrarily large distance. Certainly this is not the case for a cohesive and coherent flock by definition. Moreover, we will see in the following that for most of the stationary states, the neighboring agents indeed remain within the close proximity of an agent.

3. Random Geometric Graphs

At the initial stage N agents are uniformly distributed at random locations within a unit square box on the xy plane without periodic boundary condition. A RGG [20] is constructed whose vertices are the agents. At the same time for any arbitrary pair of vertices i and j, j is defined as a neighbor of i if it is among the n vertices nearest to i. Then an edge is assumed to exist from i to j. This implies that the edges are in general “directed” since if j is the neighbor of i then i may or may not be the neighbor of j. Therefore the resulting graph is inherently a directed graph. However, one can also define a simplified version of the graph by ignoring the edge directions and consider the graph as an undirected graph. In the following we refer such an undirected graph as the RGG.

In Figure 2 we exhibit the pictorial representation of an undirected RGG for N = 1000 as n is increased step by step. For small values of n the graph has many different components. As n is increased the components grow gradually in size, merge into one another and finally the RGG becomes a single component connected graph covering all vertices for a certain value of n. Here we have shown four figures for n = 1, 2, 3, and 4. The randomly selected positions of all vertices are exactly the same in these figures. The size of a component is measured by the number of vertices in that component. In this figure the RGG becomes fully connected for n = 4.


Figure 2. The undirected RGG with N = 1000 nodes distributed randomly within a square box with a free boundary condition. Each node is linked to its n nearest neighbors; n = 1, 2, 3, and 4 increasing from left to the right. For small n there are many components of the graph which merge with one another as n increases. The largest component has sizes 9, 150, 988, 1000.

The structure and connectivity of RGG depend on the initial positions of N vertices. Therefore we have first studied how the fraction g(N, n) of connected graphs grows with n when the flock size N is increased. For a particular RGG the connectivity is checked using the “Burning Algorithm” [21] where the fire, initiated at an arbitrary vertex, propagates along the edges and finally burns all vertices if and only if the RGG is a single component connected graph.

In Figure 3 we show the plots of g(N, n) against n for different values of N. To find out if a minimum value of the neighbor number n exists, one can artificially prepare a linear initial configuration of agents where each agent has it's right neighbor as the nearest one. This corresponds to n = 1 but occurrence of such a configuration by random selection of positions of the agents is extremely improbable. Numerically we find that for small n the g(N, n) takes vanishingly small values. However, on increasing n, g(N, n) increases very rapidly and when n is around 7, g(N, n) ≈ 1 i.e., nearly all configurations become connected. With increasing flock size N the curves slowly shifts to higher values of the neighbor number n.


Figure 3. The fractions g(N, n) of single component connected graphs, in a sample of 1000 RGGs, are plotted against n. For N agents this fraction grows as the number of neighbors n is gradually increased. System sizes N are 256 (black), 512 (red), 1024 (green), 2048 (blue), and 4096 (magenta), increased from left to right. The number of independent configurations used for each value of n is 1000.

Only those flocks whose RGGs are single component connected graphs are considered for their dynamical evolution. In case of the slowest refreshing rate of the IZ, the initial neighbor list is maintained for the entire dynamical evolution of the flock and is never updated even if all n initial neighbors of an agent no longer remain nearest neighbors as time evolves. This means that the set of agents' velocities {vi(t + 1)} is fully determined using the detailed knowledge of the set {vi(t)}. Implication of this is, the positions and velocities are completely decoupled during the time evolution since the actual positions of agents do not play any role to determine the velocities. Therefore the topological connectivity of RGG remains invariant and is a constant of motion.

4. Stationary States

4.1. Single Sink States

Initially the N agents are randomly distributed with uniform probabilities within the unit square box on the xy plane. If the corresponding RGG is fully connected then all agents are assigned the same speed v but along different directions. The angles θi of the velocity vectors with respect to +x axis are assigned by drawing them randomly from a uniform probability distribution between 0 and 2π. As time proceeds the agents soon come out of the initial unit square box and spread out in the open two dimensional space. After some initial relaxation time the flock arrives at the stationary state. One of the most common stationary state is the one where the flock is completely coherent and cohesive. The entire flock moves along the same direction without changing the flock's spatial cohesive shape and therefore θi(t) = C for all i and are independent of time. We call these states as the “Single Sink States” (SSS). Therefore this stationary state is a fixed point of the dynamical process. A picture of such a flock has been shown in Figure 4A.


Figure 4. Flocks of size N = 512 and n = 10, moving with the speed of v = 0.03 without noise. (A) Single sink state: the fully cohesive and coherent motion of the flock is exhibited by its position at three different instants: 10,000 (blue), 11,000 (green), and 12,000 (magenta). Three straight line trajectories of individual agents are also shown. The frame size is 90 × 90 units. (B) Cyclic state: the stationary state pulsating flock has been shown at different time instants: 173,000 (black), 176,000 (red), 180,000 (green), 188,000 (blue), 192,000 (brown), 197,000 (violet), and 200,000 (magenta). The time period is 28,835. Two individual agents' circular trajectories with radius ≈ 137.67 are also shown. The frame size is 600 × 600 units.

4.2. Cyclic States

In CS the velocity directions θi of all agents change at a constant rate in absence of noise. Therefore the angular velocity θ˙i(t) = D for all agents is a constant of motion. Each agent moves in a circular orbit of its own depending on its initial position, but their radii and time periods are the same. Consequently the magnitude of the resultant velocity of the whole flock in the CS has also a constant value but its direction changes with the same angular velocity. In addition typically the shape of the flock is another circle though with some irregularities and interestingly its radius changes periodically with the same period of individual agents. Therefore the whole circular flock pulsates, i.e., periodically expands and contracts where each agent moves on its own fixed circular trajectory. We explain this motion in Figure 4B by plotting the flock at different instants of time and also show two individual agent trajectories.

For an arbitrary CS, let the probability that the radius of individual agent's circular trajectory between R and R + dR be P(R)dR. Given that the uniform speed of the agents is v and their angular velocities are θ˙, the radius of the circular trajectory is R = v/θ˙. We have studied a large number of such CS and measured the radii of the agents' orbits. In Figure 5 we show the probability distribution of these radii which follows a power law distribution P(R) ~ R−τ with τ = 1.99(2).


Figure 5. The probability distribution of the radii of the individual agent's circular orbits in the cyclic states. The power law has an exponent of τ = 1.99(2).

Throughout this paper we have used only one value of the agent speed, i.e., v = 0.03. If the speed is reduced by a certain factor a CS state remains CS but all the characteristic lengths are reduced by the same factor. The radius of the circular orbit of every agent and also the size of the flock are reduced by the same factor, the time period remaining the same. Therefore it appears that even in the continuous limit of v → 0, the characteristic features of the flocks reported here remain same.

Starting from the initial state, when the random positions and velocities are assigned to all agents, the fractions of stationary states that exhibit the SSS and CS are estimated and are denoted by gSSS(N, n) and gCS(N, n), respectively. In Figure 6 these two quantities are plotted against the neighbor number n for different flock sizes N. For a certain N, gSSS(N, n) gradually increases with increasing n (Figure 6A). For a given flock size N, however large, if the neighbor number n is increased to N − 1, then on using the dynamics mentioned in Equation (1) the stationary state flock must be both cohesive and perfectly coherent i.e., gSSS(N, N − 1) = 1. No stationary state other than SSS can exist in this limiting situation. On the other hand when n < N − 1 but n is increased, then gSSS(N, n) also gradually increases and approaches the value of unity for any arbitrary value of N. At the same time, gCS(N, n) decreases with n for a fixed N but increases with N for a fixed n (Figure 6B). Finally in Figure 6C we plot the sum gSSS(N, n) + gCS(N, n) which is less than unity for small n, but on increasing n, this sum gradually increases and reaches ≈ 1 for n = 8 for all N. It is therefore concluded that if the neighbor number is increased all other states gradually disappear and only SSS and CS states mostly dominate but ultimately for even larger value of n, it is the SSS state that only survives.


Figure 6. The occurrence of two most prominent stationary states when the neighbor number n has been varied over a range from 5 to 10 and for different flock sizes N = 64 (black), 256 (red), 512 (green), and 1024 (blue). (A) The fraction gSSS(N, n) of SSS has been plotted against n. (B) The fraction gCS(N, n) of CS has been plotted against n. (C) The sum gSSS(N, n) + gCS(N, n) has been plotted and it is seen that beyond n ≈ 8 the sum is approximately unity.

4.3. Other States

In addition there are a number of other stationary states, few of them are described below, but the list may not be exhaustive.

(1) Each agent has a constant velocity but their directions are different for different agents. For example the i-th agent has its direction of velocity θi = Ci. In this case the agents, after some relaxation time, moves outward radially. The shape of the flock is approximately circular, again with some irregularities, and the radius of the flock increases at a uniform rate. We call these states as the “Distributed Sink States” (DSS). In Figure 7A an example of the DSS has been shown. The position of the flock is shown at t = 500,000 and three agents' trajectories have been shown using different colors.


Figure 7. Flocks of size N = 512 and n = 5, moving with the speed of v = 0.03 without noise. The positions of the agents are marked by black dots and three individual agent's trajectories are shown in each case by red, blue, and magenta colors. (A) Distributed sink state: every agent moves along a fixed direction θi = Ci of its own which is different in general from the directions of motion of other agents. (B) Cycloid state: in the stationary state the trajectory of each agent is a cycloid. (C) Space-filling state: the trajectory of an agent never repeats itself but gradually fills up the space between two concentric circles. The frame sizes are 40,000, 15,000, and 350 units, respectively.

(2) In another type of stationary state, the trajectories of the individual agents are very similar to cycloids. Each agent moves radially outward in a nearly cycloidal motion (Figure 7B). A considerable number of agents form a flock of circular shape but others are scattered around this circular flock. We call these as “Cycloid States.”

(3) Thirdly, there can be rosette type stationary states. The trajectory of each agent is like a rosette which never closes and lies between two concentric circles. Consequently in the long time limit the trajectories fill the space between the two circles. This means that the mean separation between consecutive intersections of the agent trajectory with a radial section gradually vanishes as the trajectory evolves for a longer time. We call these as “Space-Filling States.” Three such rosette trajectories and the position of the flock have been shown in Figure 7C.

Few points may be mentioned here about the characteristics of the different stationary states. For example a possible anisotropic effect on the stationary states may exist due to the choice of the unit square box for releasing the agents. Initially the positions of the agents are selected randomly within unit square box on the two dimensional plane. We have compared that if the agents' locations are selected randomly within a circle of radius 1/2, no appreciable change have been observed in the fractions of different stationary states.

The center of mass of the entire flock has different kinds of trajectories in different stationary states. In SSS, the center of mass moves in a straight line exactly similar to all other agents. In CS, the trajectory of the center of mass is also a circle, but it's radius is not the same as the radius of the orbit of the individual agents, but it is some what larger. In DSS, the dynamics of the center of mass is similar to that of the agents. Although, the shape of the flock is approximately circular, but the fact that, at any instant the positioning of the agents on the circumference is not uniform, makes the center of mass move radially outward in a straight line. Motion is indeed unbounded. In cycloid states, the trajectory of the center of mass is also a cycloid and radially outward. The motion here is also unbounded. In space filling states, the trajectory of the center of mass is rosette type. In this case the trajectory is bounded.

How sensitive are the final stationary states on the choice of the random initial values of {xi, yi} and {θi} for the N agents? To study this point, we tried with a flock that evolves to a CS from a certain initial configuration. Now we again evolve the same flock, but this time we slightly change the initial configuration randomly by xi = xi + a.10−4.r and yi = yi + a.10−4.r where r is a random number. The directions {θi} of the velocity vectors are maintained the same. We then tune a, and found that with 0 < a < 1.70 the stationary state is still a CS, but with different values of the orbit radius. When a ≥ 1.75 the stationary state becomes SSS. We conclude that with some amount of perturbation the character of the stationary state remains same, but with even stronger perturbation the stationary state changes.

A preliminary calculation with our model in three dimensions shows the following features. In general, to obtain connected graphs, the value of n needs to be large compared to what is required in two dimensions. Almost always the dynamics leads to a SSS in the steady state. We did not find any other state starting from random initial conditions.

5. Dynamics in Presence of Noise

Studying the role of noise on the dynamics of the flock is very crucial. It is assumed that every agent makes a certain amount of error in judging the angle of its velocity vector at each time step. More precisely given the angles θ(t) of velocity vectors of all n + 1 agents within the IZ at time t, it first calculates the resultant of these vectors using the Equation (1). It then tops up this angle by a random amount ζ(η) which is uniformly distributed within {−η/2, η/2}. Therefore the modified Equation (1) reads as:

θi(t+1)=tan1[Σjsinθj(t)/Σjcosθj(t) ]+ζ(η).(2)

The role of the noise is to randomize the deterministic dynamics and quite expectedly the stationary state structures of the flocks exhibited in the SSS and CS patterns are gradually lost. We have studied the effect of noise on both these states by gradually increasing the strength of the noise η. In both cases we use a flock of N = 512 agents, each of them interacts with n = 10 nearest neighbors and travel with speed v = 0.03. Initially all of them are released within the square box of size unity. We first run the dynamics without any noise i.e., η = 0 and ensure that the stationary state pattern is indeed a single sink state. As the dynamics proceeds we calculate the maximal distance Rm(t) and the average distance Ra(t) of an agent from the center of mass (xc(t), yc(t)) of the flock. In Figure 8A we plot these two quantities against time and they are exactly horizontal curves which are the signatures of the SSS state. These simulations are then repeated for η > 0 and the variations of Rm(t) and Ra(t) have been shown in Figures 8B–D for η = 0.2, 0.5, and 1, respectively. In all four cases the flock starts with the same positions and velocities of the agents. It is seen that on increasing the strength of noise the stochasticity gradually sets in and the variations of Rm(t) and Ra(t) gradually become random. A similar plot has been exhibited in Figure 9 for the CS but for only a single flock. The Figure 9A shows the zero noise case and the curves are periodic. However, when the noise level is increased (Figures 9B,C) it distorts the periodicity. With small values of η, the variations are slightly distorted from the periodic variations, however, with larger strength of noise the distortion is much more. Finally for η = 1 the fluctuations look random and similar to those in the SSS (Figure 9D).


Figure 8. Effect of noise is exhibited on a single flock (N = 512 agents, each having n = 10 neighbors) which goes to a single sink state without any noise. Variation of the maximal radius Rm (blue) and the average radius Ra (red) have been shown with different strengths of the noise parameter: (A) η = 0, (B) 0.2, (C) 0.5, and (D) 1. The initial positions and velocities are same in all four cases.


Figure 9. Effect of noise is exhibited on a single flock (N = 512 agents, each having n = 10 neighbors) which goes to a cyclic state without any noise. Variation of the maximal radius Rm (blue) and the average radius Ra (red) have been shown with different strengths of the noise parameter: (A) η = 0, (B) 0.2, (C) 0.5, and (D) 1. The initial positions and velocities are same in all four cases.

Next we calculated the mean square displacement 〈r2(t, η)〉 from the origin as time passes. The averaging has been done for a single agent within a flock and over many such independent flock samples. The noise strength has been varied over a wide range of values. In Figure 10 we have displayed the variation of 〈r2(t, η)〉 against the time t using a log − log scale for six different values of η. Here again we consider flocks with fully connected RGGs. On the other hand with zero noise these configurations may lead to any of the possible stationary states. Simulating up to a maximal time of T = 108 we observed a cross-over behavior in the mean square displacement. When η is very small 〈r2(t, η)〉 ~ t with κ ≈ 1 which implies that the flock maintains a ballistic motion at the early stage, i.e., the coherence is still maintained during this period. On the other hand after a long time one gets κ = 1/2 which indicates the diffusive behavior. This implies that even if a little noise is applied for a long time, the effect of the noise becomes so strong that the flock can no longer maintain a cohesive and coherent structure any more and agents diffuse away in space. Therefore for any value of η there is a cross-over from the ballistic to diffusive behavior. Consequently a cross-over time tc(η) can be defined such that for short times t << tc(η) the dynamics is ballistic with κ = 1 and for t >> tc(η) the dynamics is diffusive with κ = 1/2. In Figure 10 we show this behavior and observe that the crossover time depends explicitly on the value of η and diverges as η → 0. The value of tc(η) has been estimated by the time coordinate of the point of intersection of fitted straight lines in the two regimes of Figure 10: for t << tc(η) and for t >> tc(η). The value of tc(η) so estimated diverges as tc(η) ~ η−2.52.


Figure 10. The mean square displacement 〈r2(t, η)〉 of an agent from the origin has been plotted against time for different values of the noise parameter η = 0.2 (black), 0.5 (red), 1.0 (green), 2.0 (blue), 3.0 (magenta), and 4.0 (brown). The flock size N = 512 and the neighbor number n = 10. Two short straight lines are the guides to the eye whose slopes are κ = 1/2 and 1.

This transition is more explicitly demonstrated using a plot of the Order Parameter (OP) M(η) against η (Figure 11). The OP is defined as the time averaged magnitude of the resultant of all agents' velocity vectors, scaled by its maximum value


where 〈…〉 denotes the time average over a long period of time in the stationary state. In Figure 11A we have plotted M(η) against η at an interval of Δη = 0.1 for different system sizes from N = 64 to 1024. In these simulations the initial conditions are chosen to be completely coherent so that the velocity vectors of all agents are in the same direction. In the absence of noise this situation is maintained and M(0) = 1 at all times for all system sizes. However, for η > 0 noise sets in, but in the stationary state one still gets a non-zero OP. On further increasing η the OP decreases monotonically and ultimately vanishes. Therefore there exists a critical value ηc(N) of the noise parameter where the transition from the ordered state to disordered state takes place. It is observed in Figure 11A that as the system size N is enlarged the transition becomes more and more sharp and shifts to the regime of small η. Further we have calculated the Binder cumulant G(η) = 1 − 〈M4(η)〉/3〈M2(η)〉2 and plotted against η in Figure 11B for the same system sizes [22]. The value of G(η) drops from a constant value of around 2/3 at the small η regime to about 1/3 for large values of η.


Figure 11. (A) The stationary state order parameter M(η) and (B) the Binder cumulant G(η) have been plotted for the system sizes N = 64 (black), 128 (red), 256 (green), 512 (blue), and 1024 (magenta) where all agents start with their initial velocities in the same direction. System size increases from right to left. (C) Extrapolation of ηc(N) values determined from (A) and (B). We obtained ηc(N) = 1.70 + N−1/2.86 and ηc(N) = 1.82 + N−1/3.50, respectively.

The transition point ηc can be estimated in the following two ways. For each curve in Figure 11A we calculate the value of η1/2(N) for which M(η) = 1/2. We define η1/2(N) to be the characteristic noise level where the transition takes place. By interpolation of the plots in Figure 11A of the points around M(η) = 1/2, we have estimated η1/2(N). These estimates are then extrapolated in Figure 11C as:


On tuning the trial values of ν very slowly we found that for ν ≈ 2.86 the error in the least square fit of the above finite-size correction formula is minimum. Therefore the extrapolated η1/2(∞) ≈ 1.70 is the critical noise strength ηc according to our estimate. A similar calculation has also been done using the Binder cumulant. From this calculation we estimated ηc = 1.82 and ν = 3.50. The differences between the two estimates are considered as the error in the measured values which are 0.12 and 0.64 for ηc and ν, respectively.

Since the agents are uniformly distributed initially, the edges of RGG also are homogeneously distributed as shown in Figure 2 for n = 4. However, with time evolution these edges change their positions but their connectivity do not change, i.e., the end nodes of every edge are always fixed since the neighbor list does not change. How they look in the stationary state has been exhibited in Figure 12. This is the picture of the circle shaped flock in the cyclic state. The blue dots represent the agents and the red lines represent the edges. What is interesting to note is that the system self-organizes itself so that not only agents but also the edges are constrained to be within a very limited region of the space. Very few edges criss-cross the flock from one side to the opposite side. Initially each agents had its n neighbors at its closest distances. After passing through the relaxation stage and arriving at the stationary state, when the shape of the flock is completely different from its initial shape, most of the agents maintain their connections with other agents in their local neighborhood only.


Figure 12. The position of a flock (N = 512, n = 10) in CS by blue dots and links by red lines. The frame size is 150 units.

6. The Fastest Refreshing Rate of the Interaction Zone

Here we consider the case corresponding to the fastest refreshing rate of the IZ, i.e., when every agent updates its n nearest neighbors at every time step. Consequently, the RGG is no longer a constant of motion in this case and is updated at each time step. While performing simulations of this version, we first notice that in the long time stationary state the entire flock becomes fragmented with probability one into different clusters. For a flock of N agents with neighbor number n, the minimum number of agents in a cluster is n + 1. An agent of a particular cluster has all n neighbors which are members of that cluster only. In the stationary state all agents of a cluster has exactly the same direction of velocity and the entire cluster moves along this direction with uniform speed v. Therefore, the velocity direction θ of a particular cluster can be looked upon as the identification label of that cluster. The shape of the flock is approximately circular since each cluster travels outward with same speed (Figure 13A). Moreover, within a cluster if the agent i is a neighbor of the agent j then j is also a neighbor of i. Therefore the sub-graph of the entire RGG specific to a cluster is completely undirected and the corresponding part of the adjacency matrix is symmetric (Figure 13B). This immediately implies that the N × N adjacency matrix of the entire flock can be written in a block-diagonal form by assigning suitable identification labels of different agents.


Figure 13. (A) Positions of a flock of N = 512 agents with n = 5 neighbors in the interaction zone and at four different time instants: 100 (black), 200 (red), 300 (green), and 400 (magenta). The RGG has been updated at every time step. Three individual agents' straight line trajectories have also been shown. There are a total of 29 clusters. (B) The sub-graph of the RGG corresponding to a specific cluster of 16 agents have been shown. An arrow has been drawn from the agent i to the agent j if j is one of the n neighbors of i. There are a total of (16 × 5) / 2 = 40 distinct links and each link is directed in both directions. It may also be noted that whole set of links are restricted to the nodes of the cluster only.

A natural question would be how the frequency distribution D(s) of different cluster sizes depends on the cluster size s. To answer this question a large number of independent flocks have been simulated and each of them was evolved to its stationary state. In the stationary state the sizes of the individual clusters are measured using the burning method. In Figure 14A a plot of D(s) vs. s for s > n has been shown on a semi-log scale for N = 512 and n = 5, the data being collected using a sample size of 20,000 independent flocks. Apart from some noise at the tail end and a maximum around the smallest value of s the plot fits well to a straight line, implying an exponentially decaying form of the frequency distribution. We conclude D(s) ~ exp(−s/sc) where sc ≈ 7.2(1).


Figure 14. (A) The frequency distribution D(s) of the cluster sizes s seems likely to have an exponentially decaying form exp(−s/sc) where sc ≈ 7.2. (B) The inset shows the plot of the average cluster size 〈s(N, n)〉 for N = 512 and n = 5 with neighbor number n on a log − log scale: N = 128 (blue), 256 (green), and 512 (red). In the main plot the vertical axis has been scaled by N1.1 which leads to a data collapse.

Next, the average number of clusters 〈ns(N, n)〉 has been calculated and plotted in the inset of Figure 14B for N = 128, 256, and 512 and n = 5 on a log − log scale. Again, apart from the tail end, the plots fit very nicely to parallel straight lines, the slopes of which are estimated to be 1.168(5). In the main part of Figure 14B a scaling has been shown which exhibits a nice data collapse, corresponding to the following form


This implies that as the neighbor number n increases, there would be fewer clusters in the stationary state. On the other hand, for a specific value of n, the average cluster number grows with the flock size as N1.1. Assuming that the above scaling relation holds good for the entire range of n, for a given N one can define a cut-off value of n = nc such that 〈ns(N, nc)〉 = 1 which leads to nc(N) ~ N1.1/1.168 = N0.94. However, our simulations suggest that due to the presence of an upward bending at the tail end, the above scaling relation does not work at this end and nc(N) is actually of the order of N.

7. Vortices on the Square Lattice

In this section we studied a simpler version of our model where every agent is a spin vector. They are no more mobile, their positions are completely quenched at the sites of a regular lattice, but the directions θi(t) of the spins are the only dynamical variables that evolve with time following Equation (1). More specifically, spins are placed on a square lattice with different choices for the first n neighbors and we study the spatio-temporal patterns that emerge during the time evolution of the angular variables {θi(t)}. The arrangement of the spins allows to draw a parallel with the dynamics of planar spins in the two dimensional XY model.

The connections between the Vicsek model [8] and the 2d XY model [23] have been explored since long [3, 19, 24]. It is well known that in the limit of speed v → 0 the dynamics of the Vicsek model would exactly map on to the finite temperature Monte Carlo dynamics of the 2d XY model. However, in the latter model any long-range ordered phase is absent. Instead a quasi-long-range ordered phase appears at the low temperatures and the transition to the disordered phase is associated with the simultaneous unbinding and increase of vortex-antivortex (VAV) pairs. In the low temperature phase VAV pairs are to be found in tightly bound states. We find that our model defined on the square lattice also gives rise to VAV pairs and we determine the density of such pairs, as a function of the noise amplitude η.

We define the IZ of an agent with respect to its n nearest neighbors on the square lattice of size L × L with the periodic boundary condition. For n = 2, the IZ includes the top and the right nearest neighbors. For n = 3, the left nearest neighbor is also included and in the case of n = 4, all the four nearest neighbors are included. We notice that our model for the n = 4 case and the Vicsek model, with spins similarly placed on the square lattice, are the same. As before we study the dynamics of the spin system with and without noise.

In the absence of noise, beginning from arbitrary initial conditions for θi's, the dynamics results in the formation of VAV pairs. For n = 2 and 3, the interactions are anisotropic. Consequently the entire spin pattern in the stationary state as well as all VAV pairs are mobile and in general all the spin orientations θi's change with time. In comparison, for n = 4, all the θi's remain frozen in time which also implies that all the VAV pairs are anchored. We find that the choice of the IZ, in addition to the periodic boundary condition, fixes the direction of motion of the VAV pairs. In the Figure 15A an instantaneous configuration of the spins is plotted for a lattice with L = 64 and n = 2. In general for the n = 2 case the entire spin pattern moves on the average along the diagonal direction from top-right to bottom-left. For the case, n = 3, the vortices travel from the bottom to the top.


Figure 15. (A) Vortex-antivortex pairs of the spin systems in the stationary state in a square lattice with size L = 64 and n = 2 with zero noise. The orientations of the spins change with time in such a way so that the entire spin pattern with vortices and the antivortices move with a uniform speed from the top-right corner to the bottom-left corner. Vortices and antivortices are marked by filled red and blue circles. (B) The number V(0, L) of vortex-antivortex pairs at zero noise for different values of n in lattices of three different sizes: L = 32 (circles), 64 (squares), and 128 (triangles). The bars indicate the standard deviation in the values obtained from around 100 configurations in each case. In the inset the percentage of configurations which lead to steady states with vortex pairs is plotted against n.

Let the V(η, L) be the number of VAV pairs observed at noise η in lattice of size L. The number of VAV pairs observed at zero noise, V(0, L) is plotted against the value of n in the Figure 15B for different lattice sizes. We observe during the time evolution for a given initial condition that the number of VAV pairs initially decays and then becomes stationary. However, different initial conditions leads to different values at the stationary states. The bars indicate the dispersion that is observed for different initial conditions which lead to non-zero number of VAV pairs. For the lattice size L = 128 we wait for 105 steps before calculating number of VAV pairs. The inset to the Figure 15B shows the percentage of initial conditions that lead to non-zero number of VAV pairs. We find as lattice size increases, arbitrary initial conditions, almost always, lead to states with VAV pairs.

The nature of the time variation of the spin angle θi's for the cases n = 2 and n = 3 are found to be quite complex. In the Figure 16A we plot the time series corresponding to the oscillation of the x-component of a typical spin vector for L = 64 and n = 2. The corresponding power spectrum apparently reveals the presence of three basic frequencies f0, f1, and f2 all of which are rational multiples of 1/L (Figure 16B). The time evolution can be explained as a periodic oscillation with f1 and f2 (since f2 = 2f1) riding on a very slow mode. These features carry over to L = 128 as well. We find that in the case of n = 3, the spectrum is similar but the frequencies are not simple multiples of 1/L.


Figure 16. (A) The x-component of a typical spin vector is plotted against time for lattice with L = 64 and n = 2 at zero noise. (B) The corresponding power spectrum indicates the presence of three basic frequencies f0 = 1/(4096L), f1 = 1/(3L), and f2 = 2/(3L). The higher frequencies can be expressed as combinations of the f1 and f2 and essentially become harmonics of f1 since f2 = 2f1.

It is known that metastable vortices are produced at low temperatures in the 2d XY model when equilibrium is achieved beginning from arbitrary initial conditions. However, these vortices are not responsible for the VAV unbinding transition [25]. Therefore, we study the effect of noise by “cooling down” [26] the system to zero noise level starting from a high value of noise. At each noise level the system initially passes through 105 time steps; after this relaxation it passes through an additional 104 time steps and then moves to the next lower level of noise. We begin around the value of noise given by η = 3.7 and decrease η by an amount 0.07 in each step. This method suppresses the generation of the VAV pairs at low noise. At zero noise the vortices are absent in contrast to the statistics discussed in the previous paragraphs where the cooling down method was not employed.

At zero noise we find the spin system reaches the globally ordered state where all the spin vectors are oriented in the same direction. We believe that this is due to the finite size effect of the lattice. The spin configuration at low noise of η = 0.15 has been shown in the Figure 17A for L = 64 and n = 4 where not only vortices are absent but the long-range order is also not present. At the higher noise levels VAV pairs start appearing and there is a rapid increase in the number of pairs with further increase in noise. All the VAV pairs appearing initially are tightly bound i.e., lattice spacing is small between the members in a pair as in Figure 17B) but at higher noise members in a pair are seen to unbound (Figure 17C).


Figure 17. The figure shows proliferation of vortices as noise is increased in a square lattice of length L = 64 with n = 4. (A) For η = 0.15 there are no vortices, (B) for η = 0.35 vortices begin to appear, there are only two vortex-antivortex pairs, and (C) for η = 0.40 twenty one vortex-antivortex pairs can be seen. Filled circles of two different colors, red for vortices and blue for antivortices, have been drawn around the vortex centers.

The OP M(η) tends to unity as η → 0 as shown in the Figure 18A. In Figure 18B we plot the vortex-pair density, defined as ρ = V/L2. The natural collapse of the plots belonging to different system sizes indicates a functional dependence of ρ on n and η, which is independent of L. To understand this behavior we obtain the collapse of ln(1/ρ(η, L)) vs. nγ/η with γ = 0.28 in Figure 18C for different values of L and n. The plot reveals that in the region where VAV pairs start proliferating ρ~exp(Anβηα), where A, β, and α are constants. We estimate α by averaging slope of individual curves which yields α = 2.68 ± 0.13. This gives β = γα = 0.75. This result is in contrast to the relation ρ~exp(aT), where a is VAV pair energy and T is the temperature for the 2d XY model [26].


Figure 18. The behavior of different quantities against noise for lattice sizes L = 32 (black), 64 (red), and 128 (green) with values of n = 2 (circle), 3 (square), and 4 (triangle). (A) The variation of the order parameter M(η, L) against noise η are shown for L = 128 and for n = 2, 3, and 4. (B) The vortex-pair density ρ(η, L) against η. (C) Scaling collapse of ln(1/ρ(η, L)) against nγ/η. For the collapse we use γ = 0.28. The dashed straight line, having slope α = 2.68, is a guide for the eye and indicates the power-law nature in the low noise regime.

8. Summary and Discussion

To summarize, we have studied a simple model of the collective behavior of N interacting mobile agents which travel in the open free space. In this model we have incorporated the observation of the StarFlag experiment which advocates the necessity of using the topological distance instead of the metric distance. Each agent interacts with a group of n selected agents around it who are positioned within an IZ. Every agent freshly selects at a certain rate the group of agents within the IZ. The selection criterion is to choose the first n neighbors. In this paper we have studied two limiting situations, i.e., when the refreshing rates are fastest and the slowest. We first studied when the refreshing rate is slowest i.e., when the IZ for each agent is determined at the beginning and is never updated. All the agents follow the interaction rule in Vicsek model. It has been observed that in absence of noise, starting from a small localized region of space the agents gradually spread as time passes, so that after some relaxation time the flock arrives at a stationary state. The most prominent stationary states are the single sink state and the cyclic state. Using numerical methods we claim that the frequencies of occurrence of other stationary states like the DSS, cycloid states and the space-filling states goes to zero as the neighbor number increases to about 8. Beyond n = 8 only the SSS and CS states dominate. Finally as n approaches the flock size N, only the SSS states dominate.

Interestingly, it has also been observed that the actual metric distances of the n topological neighbors do not become arbitrarily large in all these stationary states in absence of noise. For the SSS states it is true exactly. For the CS also the topological neighbors remain within a finite distance from an agent (see Figure 12). Moreover, when the refreshing rate is the fastest, every fragmented cluster travels in a single sink state. Therefore, it is this close proximity of the neighbors that gives rise to the cohesiveness present in our model.

Further, on the application of noise a crossover takes place from the ballistic motion to the diffusive motion and the crossover time depends on the strength of the noise η, which diverges as η → 0. Further the calculation of the OP M(η) and the Binder cumulant G(η) lead us to estimate the critical noise ηc required for the continuous transition from the ordered to the disordered phase. Secondly, when the refreshing rate is fastest, each agent freshly determines its neighbors in the IZ at every time step. In the stationary state the flock gets fragmented into a number of smaller clusters of different sizes. The agents in a cluster move completely coherently, different cluster has different direction of motion.

A simpler version of the model has also been studied in the limit of the speed v → 0 when the positions of spins are completely frozen at the sites of a square lattice, but their orientational angles θi(t) evolve with time again by the Vicsek interaction. Here for n = 4 the spin configuration is completely static. On the other hand for n = 2 and 3, the entire spin configuration moves along the diagonal and parallel to the asymmetry axis, respectively. Further we have observed that the density of vortex-antivortex pairs increases with the strength of the noise and fits to a nice finite-size scaling behavior.

Overall, our findings suggest that complex spatio-temporal patterns may emerge in the interplay between an underlying network structure and collective motion. We believe that our study would also be relevant in the general problem of consensus development in networked agents [27] and as such issues like undesired synchronization observed in real-world networks [28]. We observed that multiple frequencies develop during oscillations of different dynamical variables. Whether there is a possibility that a cascade of frequencies develop eventually leading to chaotic behavior remains an open question.

Conflict of Interest Statement

The authors declare that the research was conducted in the absence of any commercial or financial relationships that could be construed as a potential conflict of interest.


Useful discussion with Shraddha Mishra is thankfully acknowledged. Kunal Bhattacharya acknowledges the support from the BITS Research Initiation Grant Fund.


1. Reynolds CW. Flocks, herds and schools: a distributed behavioral model. Comput Graph. (1987) 21:25–34. doi: 10.1145/37402.37406

CrossRef Full Text

2. Vicsek T, Zafeiris A. Collective motion. Phys Rep. (2012) 517:71–140. doi: 10.1016/j.physrep.2012.03.004

CrossRef Full Text

3. Toner J, Tu Y. Long-range order in a two-dimensional dynamical XY model: how birds fly together. Phys Rev Lett. (1995) 75:4326–9. doi: 10.1103/PhysRevLett.75.4326

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

4. Buhl J, Sumpter DJT, Couzin ID, Hale JJ, Despland E, Miller ER, et al. From disorder to order in marching locusts. Science. (2006) 312:1402–6. doi: 10.1126/science.1125142

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

5. Nagy M, Ákos Z, Biro D, Vicsek T. Hierarchical group dynamics in pigeon flocks. Nature. (2010) 464:890–3. doi: 10.1038/nature08891

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

6. Croft DP, Arrowsmith BJ, Bielby Skinner K, White E, Couzin ID, Magurran AE, et al. Mechanisms underlying shoal composition in the Trinidadian guppy, Poecilia reticulata. Okios. (2003) 100:429. doi: 10.1034/j.1600-0706.2003.12023.x

CrossRef Full Text

7. Moussaïd M, Perozo N, Garnier S, Helbing D, Theraulaz G. The walking behaviour of pedestrian social groups and its impact on crowd dynamics. PLoS ONE. (2010) 5:e10047. doi: 10.1371/journal.pone.0010047

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

8. Vicsek T, Czirók A, Ben-Jacob E, Cohen I, Shochet O. Novel type of phase transition in a system of self-driven particles. Phys Rev Lett. (1995) 75:1226–9. doi: 10.1103/PhysRevLett.75.1226

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

9. Grégoire G, Chaté, H. Onset of collective and cohesive motion. Phys Rev Lett. (2004) 92:025702–5. doi: 10.1103/PhysRevLett.92.025702

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

10. Chaté H, Ginelli F, Grégoire G, Raynaud F. Collective motion of self-propelled particles interacting without cohesion. Phys Rev E. (2008) 77:046113–27. doi: 10.1103/PhysRevE.77.046113

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

11. Ballerini M, Cabibbo N, Candelier R, Cavagna A, Cisbani E, Giardina I, et al. Interaction ruling animal collective behavior depends on topological rather than metric distance: evidence from a field study. Proc Natl Acad Sci U S A. (2008) 105:1232–7. doi: 10.1073/pnas.0711437105

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

12. Gautrais J, Ginelli F, Fournier R, Blanco S, Soria M, Chaté H, Theraulaz G. Deciphering interactions in moving animal groups. PLoS Comput Biol. (2012) 8:e1002678. doi: 10.1371/journal.pcbi.1002678

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

13. Ginelli F, Chateé H. Relevance of metric-free interactions in flocking phenomena. Phys Rev Lett. (2010) 105:168103–6. doi: 10.1103/PhysRevLett.105.168103

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

14. Peshkov A, Ngo S, Bertin E, Chaté H, Ginelli F. Continuous theory of active matter systems with metric-free interactions. Phys Rev Lett. (2012) 109:098101–6. doi: 10.1103/PhysRevLett.109.098101

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

15. Heupe C, Aldana M. New tools for characterizing swarming systems: a comparison of minimal models. Physica A. (2008) 387:2809–22. doi: 10.1016/j.physa.2008.01.081

CrossRef Full Text

16. Jadbabaie A, Lin J, Morse AS. Coordination of groups of mobile autonomous agents using nearest neighbor rules. IEEE Trans Autom Control. (2003) 48:988–1001. doi: 10.1109/TAC.2003.812781

CrossRef Full Text

17. Tanner HG, Jadbabaie A, Pappas GJ. Stable flocking of mobile agents, part I: fixed topology. Proc IEEE Conf Decis Control. (2003) 2:2010–5. doi: 10.1109/CDC.2003.1272910

CrossRef Full Text

18. Bode NWF, Wood AJ, Franks DW. The impact of social networks on animal collective motion. Anim Behav. (2011) 82:29–38. doi: 10.1016/j.anbehav.2011.04.011

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

19. Chaté H, Ginelli F, Montagne R. Simple model for active nematics: quasi-long-range order and giant fluctuations. Phys Rev Lett. (2006) 96:180602–5. doi: 10.1103/PhysRevLett.96.180602

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

20. Dall J, Christensen M. Random geometric graphs. Phys Rev E. (2002) 66:016121–9. doi: 10.1103/PhysRevE.66.016121

Pubmed Abstract | Pubmed Full Text | CrossRef Full Text

21. Herrmann HJ, Hong DC, Stanley HE. Backbone and elastic backbone of percolation clusters obtained by the new method of “burning.” J Phys A. (1984) 17:L261–6. doi: 10.1088/0305-4470/17/5/008

CrossRef Full Text

22. Nagy M, Daruka I, Vicsek T. New aspects of the continuous phase transition in the scalar noise model (SNM) of collective motion. Physica A. (2007) 373:445–54. doi: 10.1016/j.physa.2006.05.035

CrossRef Full Text

23. Kosterlitz JM, Thouless DJ. Ordering, metastability and phase transitions in two-dimensional systems. J Phys C. (1973) 60:1181–1203. doi: 10.1088/0022-3719/6/7/010

CrossRef Full Text

24. Toner J, Tu Y, Ramaswamy S. Hydrodynamics and phases of flocks. Annal Phys. (2005) 318:170–244. doi: 10.1016/j.aop.2005.04.011

CrossRef Full Text

25. Miyashita S, Nishimori H, Kuroda A, Suzuki M. Monte Carlo simulation and static and dynamic critical behavior of the plane rotator model. Prog Theor Phys. (1978) 60:1669–85. doi: 10.1143/PTP.60.1669

CrossRef Full Text

26. Tobochnik J, Chester GV. Monte Carlo study of the planar spin model. Phys Rev B. (1979) 20:3761–9. doi: 10.1103/PhysRevB.20.3761

CrossRef Full Text

27. Olfati-Saber R, Murray RM. Consensus and cooperation in networked multi-agent systems. Proc IEEE. (2007) 95:215–33. doi: 10.1109/JPROC.2006.887293

CrossRef Full Text

28. Floyd S. The synchronization of periodic routing messages. IEE/ACM Trans Netw. (1994) 2:122–36. doi: 10.1109/90.298431

CrossRef Full Text

Keywords: collective behavior, flocking, cyclic states, phase transition, spin model

Citation: Bhattacherjee B, Bhattacharya K and Manna SS (2014) Cyclic and coherent states in flocks with topological distance. Front. Physics 1:35. doi: 10.3389/fphy.2013.00035

Received: 18 September 2013; Accepted: 23 December 2013;
Published online: 17 January 2014.

Edited by:

Knut J. Måløy, Fysisk Institutt Universitetet i Oslo, Norway

Reviewed by:

Renaud Toussaint, University of Strasbourg, France
Osvanny Ramos, University Claude Bernard Lyon 1, France

Copyright © 2014 Bhattacherjee, Bhattacharya and Manna. This is an open-access article distributed under the terms of the Creative Commons Attribution License (CC BY). The use, distribution or reproduction in other forums is permitted, provided the original author(s) or licensor are credited and that the original publication in this journal is cited, in accordance with accepted academic practice. No use, distribution or reproduction is permitted which does not comply with these terms.

*Correspondence: S. S. Manna, Department of Theoretical Sciences, Satyendra Nath Bose National Centre for Basic Sciences, Block-JD, Sector-III, Salt Lake, Kolkata-700098, West Bengal, India e-mail: