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The velocity distribution functions of particles in one- and three-dimensional harmonic solids are investigated through molecular dynamics simulations. It is shown that, as in the case of dense fluids, these distribution functions still obey the Maxwell-Boltzmann law and the assumption of molecular chaos remains valid even at low temperatures.

In the classical theory of ideal gases, the velocity distribution function is derived from the Boltzmann transport equation based on the assumption of molecular chaos and a dilute enough gas so that ternary and higher collisions can be ignored [

However, it can be shown that the Maxwell-Boltzmann distribution function describes molecular velocities even in non-ideal gases [

In what follows, we extend this investigation to include solids with strong harmonic interactions between its particles. Solids are interesting because contrary to fluids where the particles can move throughout the entire volume available to the fluid, in solids the particles can only oscillate about their mean equilibrium positions, and for strong interactions these oscillations are restricted to a very limited region of space.

The choice of harmonic interactions between the particles is due to the fact that any interaction between particles of a solid can be approximated by a harmonic potential as long as the displacements of the particles from their equilibrium positions remain small. Of course, solids with harmonic interatomic interactions have long been studied extensively [

The normalized Maxwell-Boltzmann velocity distribution function (or probability density function) of a perfect gas in one dimension is given by [

f ( v x ) = ( m 2 π k T ) 1 / 2 exp ( − m v x 2 2 k T ) . (1)

Assuming molecular chaos, the velocity distribution function in three dimensions can be written as the product of the one-dimensional distribution functions [

f ( v x , v y , v z ) = f ( v x ) f ( v y ) f ( v z ) = ( m 2 π k T ) 3 / 2 exp ( − m v 2 2 k T ) (2)

where v 2 = v x 2 + v y 2 + v z 2 . Then the probability of finding a particle with velocity in the interval ( v x , v y , v z ) to ( v x + d v x , v y + d v y , v z + d v z ) is f ( v x , v y , v z ) d v x d v y d v z . Transforming this probability to spherical coordinates in velocity space with d v x d v y d v z = v 2 d v sin θ d θ d ϕ and integrating over q and f, we obtain the Maxwell-Boltzmann speed distribution function in three dimensions,

f ( v ) = 4 π ( m 2 π k T ) 3 / 2 v 2 exp ( − m v 2 2 k T ) . (3)

As stated above, in this work we assume a harmonic potential for interaction of the atoms. This is because any general interatomic potential energy function of two atoms can be expanded is a Taylor series about the equilibrium position of the atoms,

u ( r ) = u ( r 0 ) + 1 1 ! u ′ ( r 0 ) ( r − r 0 ) + 1 2 ! u ″ ( r 0 ) ( r − r 0 ) 2 + ⋯ (4)

where r is the distance between the two atoms and r_{0} is the equilibrium distance. The first term on the right hand side is a constant, which defines the reference of the potential energy. This constant can arbitrarily be set equal to zero. The second term is zero because the force on the particle is given by

F = − d u d r (5)

and at equilibrium the force on the particle is zero. The coefficient of the third term is positive because the potential energy is a minimum at a stable equilibrium point. Finally, for small displacements of the particles from their equilibrium ( r − r 0 ), we can ignore the higher-order terms in the expansion (4), and write

u ( r ) = 1 2 c ( r − r 0 ) 2 (6)

where c = u ″ ( r 0 ) is a positive constant. Therefore, for small deviations from equilibrium, a particle under any interatomic potential energy function in a solid experiences a harmonic potential. However, it should be pointed out that this analysis is valid as long as the potential energy function is not intrinsically nonlinear [

The interactions between atoms in many simple solids are described by Lennard-Jones (6-12) potential energy function [

u ( r ) = 4 ϵ [ ( σ r ) 12 − ( σ r ) 6 ] (7)

where ϵ and σ are constants with units of energy and length, respectively. The first term in this equation corresponds to attraction between the two atoms resulting from van der Waals interaction between them [

Differentiating Equation (7) with respect to r and setting it equal to zero gives

r 0 = 2 1 / 6 σ . (8)

A second differentiation of Equation (7) and its evaluation at r = r 0 gives

u ″ ( r 0 ) = d 2 u ( r ) d r 2 | r = r 0 = 72 ϵ 2 1 / 3 σ 2 . (9)

Therefore according to Equation (6), for small deviations from equilibrium, the Lennard-Jones potential reduces to a harmonic potential given by

u ( r ) = 1 2 ( 72 ϵ 2 1 / 3 σ 2 ) ( r − r 0 ) 2 . (10)

We investigate both a one-dimensional and a three-dimensional solid. This is because in some cases one-dimensional systems behave differently from those of higher dimensions. In addition, correlating the results of the one-dimensional system with those of the three-dimensional system can further verify the validity of the assumption of molecular chaos. Furthermore, in order to mimic an actual atomic solid in our simulations, we consider argon-like particles interacting according to a harmonic potential energy function given by Equation (10).

Since the actual atomic parameters are very small in SI units, we use a reduced system of units. In this system the mass of the atoms m is the unit of mass and the equilibrium distance between the atoms r_{0} is the unit of length. For argon, the atomic mass and the Lennard-Jones potential parameters are [

m = 6.69 × 10 − 26 kg , σ = 3.42 × 10 − 10 m , ϵ = 1.65 × 10 − 21 J . (11)

Therefore, in our system of units, the unit of mass is 6.69 × 10 − 26 kg and the unit of length (r_{0}) is 3.84 × 10 − 10 m . Finally, we take ϵ = 1.65 × 10 − 21 J and ϵ / k = 120 K to be our units of energy and temperature, respectively, where k = 1.38 × 10 − 23 J / K is the Boltzmann’s constant. This completes our system of units. Any other physical quantity in our simulations can be written as a combination of these units, as shown in

All of the simulations, in one and in three dimensions, were carried out using the velocity form of the Verlet algorithm [

{ ξ n + 1 = ξ n + v n Δ t + 1 2 a n ( Δ t ) 2 v n + 1 = v n + 1 2 ( a n + 1 + a n ) Δ t (12)

Physical Quantity | Reduced Unit | SI Value for Argon |
---|---|---|

Mass | m | 6.69 × 10 − 26 kg |

Length | r 0 | 3.84 × 10 − 10 m |

Energy | ϵ | 1.65 × 10 − 21 J |

Time | r 0 ( m / ϵ ) 1 / 2 | 2.45 × 10 − 12 s |

Speed | ( ϵ / m ) 1 / 2 | 157 m/s |

Force | ϵ / r 0 | 4.30 × 10 − 12 N |

Temperature | ϵ / k | 120 K |

with a time step of Δ t = 0.01 reduced unit, where x stands for x, y, or z, and v and a are the corresponding velocity and acceleration, respectively. Furthermore, throughout the investigation periodic boundary conditions were used to reduce the size effect of the systems.

We studied a linear chain of 200 argon-like particles, each of mass m, with spring-like interaction between the adjacent particles,

F = − c ( r − r 0 ) (13)

where r is the instantaneous distance between two adjacent atoms and r_{0} is the relaxed length of the spring. Since

F = − d u d r (14)

according to Equation (10) the constant c in Equation (13) is given by

c = 72 ϵ 2 1 / 3 σ 2 (15)

which, in our reduced system of units, has a value of 72.

The particles were initially arranged on a straight line at one unit of length intervals. Each particle was then randomly given a velocity of +1 or −1 reduced unit and then the center of mass of the system was brought to rest. The temperature of the system was calculated from

〈 K 〉 = 1 2 k T (16)

where 〈 K 〉 is the mean kinetic energy of the particles. The velocity of each particle was then re-scaled according to the following equation to adjust the temperature of the system to the desired value [

v i n e w = v i T d T a (17)

where T a is the actual temperature calculated from (16) and T d is the desired temperature.

The simulation was allowed to run for 1000 time steps to thermalize the system before any data were collected. After thermalization, data were collected on the temperature of the system as a function of time step and the velocity distribution of the particles over the next 10^{5} time steps. We also monitored the velocity of the center of mass of the system to ensure the center of mass did not drift during the simulation, or there was no “wind” in the system.

We simulated the system with temperatures of T = 0.5 and T = 1.0 reduced unit.

f ( v ) = 1 π e − v 2 (18)

and for T = 1.0 ,

f ( v ) = 1 2 π e − v 2 / 2 . (19)

These are shown as solid curves in

In this part of the investigation, we studies a system of 512 argon-like particles ( 8 × 8 × 8 ) on a simple cubic lattice, the unit cell of which is shown in

Each particle was initially given a random velocity in the interval ( − 1,1 ) in each coordinate direction. These velocities were then reduced to bring the center of mass of the system to rest. The temperature of the system was then calculated from

〈 K 〉 = 3 2 k T (20)

as before, then the velocity components of each particle were re-scaled according to Equation (17) to adjust the temperature of the system to the desired value. The system was allowed to thermalize for 5000 time steps. Then data were collected during the next 10^{5} time steps on temperature and speed distribution of the particles for T = 0.5 and T = 1.0 reduced unit.

the three-dimensional system at T = 0.5 and T = 1.0 reduced unit. The figure also shows the Maxwell-Boltzmann speed distribution functions at these two temperatures. These are obtained from Equation (3) by substituting the parameters of the system in reduced units. The results for T = 0.5 and T = 1.0 are, respectively

f ( v ) = 4 π v 2 e − v 2 (21)

and

f ( v ) = 2 π v 2 e − v 2 / 2 . (22)

These are shown by solid curves in

We also point out that in the three-dimensional case as well, each of the velocity distribution functions f ( v x ) , f ( v y ) , f ( v z ) were similar to that of the one-dimensional system shown in

As pointed out earlier, the Maxwell-Boltzmann velocity distribution function, which was originally obtained for an ideal gas, remains valid even in non-ideal gases and in the presence of long-range interactions between the particles of the system as long as the assumption of molecular chaos remains valid. Later, molecular dynamics simulations showed that even in extremely dense fluid systems with strong interactions between its particles velocity distribution of the particles is Maxwellian and the assumption of molecular chaos remains valid.

In this study we have taken the investigation one step further to include solid systems where, contrary to fluid systems, motion of the particles is very limited in space, especially at low temperatures. For the argon-like particles studied, according to

Furthermore, since Equation (3) is obtained from Equation (1) based on the assumption of molecular chaos, the fact that the velocity and the speed distribution functions in one and three dimensions are both in excellent agreement with these equations is indicative of the validity of the assumption of molecular chaos in solids, even at low temperatures.

In addition, the Maxwell-Boltzmann distribution function is obtained from the Boltzmann transport equation which, in turn, is based on the assumption of a dilute gas [

n n Q ≪ 1 (23)

where n is the particle density and

n Q = ( 2 π m k T h 2 ) 3 / 2 (24)

is the quantum concentration of the system [_{0}, therefore, n = N / V = 1 / r 0 3 . Then with T = 0.5 reduced units, we have

n n Q = N V ( h 2 2 π m k T ) 3 / 2 = 1 r 0 3 [ ( 0.164 ) 2 2 π m k ( 0.5 ϵ / k ) ] 3 / 2 = [ ( 0.164 ) 2 π ] 3 / 2 = 8 × 10 − 4 ≪ 1 (25)

Therefore, even though the system that we have investigated is a solid at low temperatures, it is still in the classical regime.

Mohazzabi, P. and Shankar, S.P. (2018) Maxwell-Boltzmann Distribution in Solids. Journal of Applied Mathematics and Physics, 6, 602-612. https://doi.org/10.4236/jamp.2018.63052