Maxwell–Jüttner distribution

In physics, the Maxwell–Jüttner distribution, sometimes called Jüttner–Synge distribution, is the distribution of speeds of particles in a hypothetical gas of relativistic particles. Similar to the Maxwell–Boltzmann distribution, the Maxwell–Jüttner distribution considers a classical ideal gas where the particles are dilute and do not significantly interact with each other. The distinction from Maxwell–Boltzmann's case is that effects of special relativity are taken into account. In the limit of low temperatures T {\displaystyle T} much less than m c 2 / k B {\displaystyle mc^{2}/k_{\text{B}}} (where m {\displaystyle m} is the mass of the kind of particle making up the gas, c {\displaystyle c} is the speed of light and k B {\displaystyle k_{\text{B}}} is Boltzmann constant), this distribution becomes identical to the Maxwell–Boltzmann distribution.

The distribution can be attributed to Ferencz Jüttner, who derived it in 1911.^[1] It has become known as the Maxwell–Jüttner distribution by analogy to the name Maxwell–Boltzmann distribution that is commonly used to refer to Maxwell's or Maxwellian distribution.

Definition

As the gas becomes hotter and k B T {\displaystyle k_{\text{B}}T} approaches or exceeds m c 2 {\displaystyle mc^{2}} , the probability distribution for γ = 1 / 1 − v 2 / c 2 {\textstyle \gamma =1/{\sqrt {1-v^{2}/c^{2}}}} in this relativistic Maxwellian gas is given by the Maxwell–Jüttner distribution:^[2]

f ( γ ) d γ = γ 2 β ( γ ) θ K 2 ( 1 θ ) e − γ / θ d γ {\displaystyle f(\gamma )\,\mathrm {d} \gamma ={\frac {\gamma ^{2}\,\beta (\gamma )}{\theta \operatorname {K} _{2}\!\left({\frac {1}{\theta }}\right)}}e^{-{\gamma }/{\theta }}\,\mathrm {d} \gamma }

where β = v c = 1 − 1 / γ 2 {\textstyle \beta ={\frac {v}{c}}={\sqrt {1-1/\gamma ^{2}}}} , θ = k B T m c 2 {\textstyle \theta ={\frac {k_{\text{B}}T}{mc^{2}}}} , and K 2 {\displaystyle \operatorname {K} _{2}} is the modified Bessel function of the second kind.

Alternatively, this can be written in terms of the momentum as f ( p ) d 3 p = 1 4 π θ K 2 ( 1 θ ) e − γ ( p ) / θ d 3 p ( m c ) 3 {\displaystyle f(\mathbf {p} )\,\mathrm {d} ^{3}\mathbf {p} ={\frac {1}{4\pi \theta \operatorname {K} _{2}\!\left({\frac {1}{\theta }}\right)}}e^{-\gamma (p)/\theta }\,{\frac {\mathrm {d} ^{3}\mathbf {p} }{(mc)^{3}}}} where γ ( p ) = 1 + ( p m c ) 2 {\textstyle \gamma (p)={\sqrt {1+\left({\frac {p}{mc}}\right)^{2}}}} . If the momentum distribution is symmetric in all 3 dimensions, the distribution can also be written in terms of the magnitude of the momentum, after integrating the 3-dimensional distribution over a sphere: f ( p ) d p = p 2 θ K 2 ( 1 θ ) e − γ ( p ) / θ d p ( m c ) 3 {\displaystyle f(p)\,\mathrm {d} p={\frac {p^{2}}{\theta \operatorname {K} _{2}\!\left({\frac {1}{\theta }}\right)}}e^{-\gamma (p)/\theta }{\frac {\mathrm {d} p}{(mc)^{3}}}}

The Maxwell–Jüttner equation is covariant, but not manifestly so, and the temperature of the gas does not vary with the gross speed of the gas.^[3]

Jüttner distribution graph

A visual representation of the distribution in particle velocities for plasmas at four different temperatures:^[4]

Where thermal parameter has been defined as μ = m c 2 k B T = 1 θ {\textstyle \mu ={\frac {mc^{2}}{k_{\text{B}}T}}={\frac {1}{\theta }}} .

The four general limits are:

• ultrarelativistic temperatures μ ≪ 1 ⟺ θ ≫ 1 {\displaystyle \mu \ll 1\iff \theta \gg 1} ( k B T ≫ m c 2 {\displaystyle k_{\text{B}}T\gg mc^{2}} ),
• relativistic temperatures: μ < 1 ⟺ θ > 1 {\displaystyle \mu <1\iff \theta >1} ( k B T > m c 2 {\displaystyle k_{\text{B}}T>mc^{2}} ),
• weakly (or mildly) relativistic temperatures: μ > 1 ⟺ θ < 1 {\displaystyle \mu >1\iff \theta <1} ( k B T < m c 2 {\displaystyle k_{\text{B}}T<mc^{2}} ),
• low temperatures: μ ≫ 1 ⟺ θ ≪ 1 {\displaystyle \mu \gg 1\iff \theta \ll 1} ( k B T ≪ m c 2 {\displaystyle k_{\text{B}}T\ll mc^{2}} ),

Limitations

Some limitations of the Maxwell–Jüttner distributions are shared with the classical ideal gas: neglect of interactions, and neglect of quantum effects. An additional limitation (not important in the classical ideal gas) is that the Maxwell–Jüttner distribution neglects antiparticles.

If particle-antiparticle creation is allowed, then once the thermal energy k B T {\displaystyle k_{\text{B}}T} is a significant fraction of m c 2 {\displaystyle mc^{2}} , particle-antiparticle creation will occur and begin to increase the number of particles while generating antiparticles (the number of particles is not conserved, but instead the conserved quantity is the difference between particle number and antiparticle number). The resulting thermal distribution will depend on the chemical potential relating to the conserved particle–antiparticle number difference. A further consequence of this is that it becomes necessary to incorporate statistical mechanics for indistinguishable particles, because the occupation probabilities for low kinetic energy states becomes of order unity. For fermions it is necessary to use Fermi–Dirac statistics and the result is analogous to the thermal generation of electron–hole pairs in semiconductors. For bosonic particles, it is necessary to use the Bose–Einstein statistics.^[5]

Perhaps most significantly, the basic MB distribution has two main issues: it does not extend to particles moving at relativistic speeds, and  it assumes anisotropic temperature (where each DoF does not have the same translational kinetic energy). While the classic Maxwell–Jüttner distribution generalizes for the case of special relativity, it fails to consider the anisotropic description.

Derivation

The Maxwell–Boltzmann (MB) distribution f MB {\displaystyle f_{\text{MB}}} describes the velocities u {\displaystyle \mathbf {u} } or the kinetic energy ε = 1 2 m u 2 = p 2 2 m {\textstyle \varepsilon ={\frac {1}{2}}m\mathbf {u} ^{2}={\frac {\mathbf {p} ^{2}}{2m}}} of the particles at thermal equilibrium, far from the limit of the speed of light, i.e.:

f MB ( p ; v th ) d n p = ( π m 2 v th 2 ) − n / 2 e − p 2 / 2 m k B T d n p , v th ≡ 2 k B T / m , f MB ( ε ; T ) d ε = ( k B T ) − n / 2 Γ ( n / 2 ) e − ε / k B T ε 1 2 n − 1 d ε {\displaystyle {\begin{aligned}f_{\text{MB}}(\mathbf {p} ;v_{\text{th}})\,\mathrm {d} ^{n}\mathbf {p} &=\left(\pi m^{2}v_{\text{th}}^{2}\right)^{-n/2}e^{-{\frac {\mathbf {p} ^{2}/2m}{k_{\text{B}}T}}}\,\mathrm {d} ^{n}\mathbf {p} ,&v_{\text{th}}\equiv {\sqrt {2{k_{\text{B}}T}/{m}}},\\[1ex]f_{\text{MB}}(\varepsilon ;T)\,\mathrm {d} \varepsilon &={\frac {\left(k_{\text{B}}T\right)^{-n/2}}{\Gamma {\left(n/2\right)}}}e^{-\varepsilon /{k_{\text{B}}T}}\varepsilon ^{{\frac {1}{2}}n-1}\,\mathrm {d} \varepsilon \end{aligned}}}

1

where the low-energy limit (non-relativistic) can be expressed as u ≪ c {\textstyle u\ll c} , or equivalently, ε ≪ m c 2 {\displaystyle \varepsilon \ll mc^{2}} . Here, v th {\displaystyle v_{\text{th}}} is the expression of temperature as a speed, called thermal speed, and n denotes the kinetic degrees of freedom of each particle. (Note that the temperature is defined in the fluid's rest frame, where the bulk speed u b {\displaystyle \mathbf {u} _{b}} is zero. In the non-relativistic case, this can be shown by using ε = 1 2 m ( u − u b ) 2 {\textstyle \varepsilon ={\frac {1}{2}}m(\mathbf {u} -\mathbf {u} _{b})^{2}} .

The relativistic generalization of Eq. (1), that is, the Maxwell–Jüttner (MJ) distribution, is given by:

f MJ ( γ ) ∝ γ 2 β ( γ ) e − γ / θ , {\displaystyle f_{\text{MJ}}(\gamma )\propto \gamma ^{2}\beta (\gamma )\,e^{-\gamma /\theta },}

2

where θ ≡ k B T / m c 2 {\textstyle \theta \equiv {k_{\text{B}}T}/{mc^{2}}} , β ≡ u / c {\textstyle \beta \equiv u/c} , and γ ( β ) = ( 1 − β 2 ) − 1 / 2 {\textstyle \gamma (\beta )=\left(1-\beta ^{2}\right)^{-1/2}} . (Note that the inverse of the unitless temperature θ {\displaystyle \theta } is the relativistic coldness ζ {\displaystyle \zeta } .^[6]) This distribution (Eq. 2) can be derived as follows. According to the relativistic formalism for the particle momentum and energy, one has

p = m c γ ( β ) β , E ( β ) = γ ( β ) m c 2 . {\displaystyle {\begin{aligned}\mathbf {p} &=mc\,\gamma {\left(\beta \right)}\,\mathbf {\beta } ,&E{\left(\beta \right)}&=\gamma (\beta )\,mc^{2}.\end{aligned}}}

While the kinetic energy is given by ε = E − m c 2 = ( γ − 1 ) m c 2 {\displaystyle \varepsilon =E-mc^{2}=(\gamma -1)\,mc^{2}} . The Boltzmann distribution of a Hamiltonian is f MJ ( H ) ∝ e − H k B T {\displaystyle f_{\text{MJ}}(H)\propto e^{-{\frac {H}{k_{\text{B}}T}}}} . In the absence of a potential energy, H {\displaystyle H} is simply given by the particle energy E {\displaystyle E} , thus:

f MJ ( E ) ∝ e − E k B T ∝ e − γ / θ {\displaystyle f_{\text{MJ}}\left(E\right)\propto e^{-{\frac {E}{k_{\text{B}}T}}}\propto e^{-\gamma /\theta }}

(Note that E {\displaystyle E} is the sum of the kinetic ε {\displaystyle \varepsilon } and rest energy m c 2 {\displaystyle mc^{2}} , ε k B T = γ −   1 θ {\textstyle {\frac {\varepsilon }{k_{\text{B}}T}}={\frac {\gamma -\ 1}{\theta }}} ). Then, when one includes the n-dimensional density of states:

f MJ ( γ ) ∝ p ( γ ) n − 1 d p ( γ ) d γ e − γ / θ {\displaystyle f_{\text{MJ}}(\gamma )\propto p(\gamma )^{n-1}{\frac {\mathrm {d} p(\gamma )}{\mathrm {d} \gamma }}\,e^{-\gamma /\theta }}

So that:

∫ f MJ ( p ) d p 1 ⋯ d p n ∝ ∫ e − E ( p ) k B T d p 1 ⋯ d p n = ∫ e − E ( γ Ω n ) k B T d Ω n p n − 1 d p = ∫ Ω n e − E ( γ Ω n ) k B T ( p ( γ ) n − 1 d p ( γ ) d γ ) d Ω n d γ {\displaystyle {\begin{aligned}\int f_{\text{MJ}}(\mathbf {p} )\,\mathrm {d} p_{1}\cdots \mathrm {d} p_{n}&\propto \int e^{-{\frac {E(\mathbf {p} )}{k_{\text{B}}T}}}\,\mathrm {d} p_{1}\cdots \mathrm {d} p_{n}\\[1ex]&=\int e^{-{\frac {E(\gamma \Omega _{n})}{k_{\text{B}}T}}}\,\mathrm {d} \Omega _{n}\,p^{n-1}\,\mathrm {d} p\\[1ex]&=\int _{\Omega _{n}}e^{-{\frac {E(\gamma \Omega _{n})}{k_{\text{B}}T}}}\,\left(p(\gamma )^{n-1}{\frac {\mathrm {d} p(\gamma )}{\mathrm {d} \gamma }}\right)\mathrm {d} \Omega _{n}\,\mathrm {d} \gamma \end{aligned}}}

Where d Ω n {\displaystyle \mathrm {d} \Omega _{n}} denotes the n-dimensional solid angle. For isotropic distributions, one has

∫ f MJ ( p ) d p 1 ⋯ d p n ∝ ∫ e − E ( p ) k B T ( p ( γ ) n − 1 d p ( γ ) d γ ) d Ω n d γ ≡ ∫ Ω n d Ω n ∫ f MJ ( γ ) d γ {\displaystyle \int f_{\text{MJ}}(p)\,\mathrm {d} p_{1}\cdots \mathrm {d} p_{n}\propto \int e^{-{\frac {E(p)}{k_{\text{B}}T}}}\left(p(\gamma )^{n-1}{\frac {\mathrm {d} p(\gamma )}{\mathrm {d} \gamma }}\right)\mathrm {d} \Omega _{n}\,\mathrm {d} \gamma \equiv \int _{\Omega _{n}}\mathrm {d} \Omega _{n}\,\int f_{\text{MJ}}(\gamma )\,\mathrm {d} \gamma }

or

f MJ ( γ ) ∝ e − E ( γ ) k B T p ( γ ) n − 1 d p ( γ ) d γ {\displaystyle f_{\text{MJ}}(\gamma )\propto e^{-{\frac {E(\gamma )}{k_{\text{B}}T}}}\,p(\gamma )^{n-1}{\frac {\mathrm {d} p(\gamma )}{\mathrm {d} \gamma }}}

Then, d ( γ β ) = γ ( γ 2 − 1 ) − 1 2 d γ = β − 1 d γ {\displaystyle \mathrm {d} (\gamma \beta )=\gamma \left(\gamma ^{2}-1\right)^{-{\frac {1}{2}}}\mathrm {d} \gamma =\beta ^{-1}\,\mathrm {d} \gamma } so that:

p ( γ ) n − 1 d p ( γ ) d γ = ( m c ) n ( γ β ) n − 1 d ( γ β ) d γ = ( m c ) n γ n − 1 β n − 2 , {\displaystyle {\begin{aligned}p\left(\gamma \right)^{n-1}{\frac {\mathrm {d} p\left(\gamma \right)}{\mathrm {d} \gamma }}&=\left(mc\right)^{n}\left(\gamma \beta \right)^{n-1}{\frac {\mathrm {d} (\gamma \beta )}{\mathrm {d} \gamma }}\\&=\left(mc\right)^{n}\gamma ^{n-1}\beta ^{n-2},\end{aligned}}}

Or:

f MJ ( γ ) ∝ γ n − 1 β n − 2 e − γ θ ∝ γ ( γ 2 − 1 ) n 2 − 1 e − γ θ {\displaystyle f_{\text{MJ}}(\gamma )\propto \gamma ^{n-1}\beta ^{n-2}e^{-{\frac {\gamma }{\theta }}}\propto \gamma \left(\gamma ^{2}-1\right)^{{\frac {n}{2}}-1}\,e^{-{\frac {\gamma }{\theta }}}}

3

Now, because E k B T = γ θ {\displaystyle {\frac {E}{k_{\text{B}}T}}={\frac {\gamma }{\theta }}} . Then, one normalises the distribution Eq. (3). One sets f MJ ( p , θ ) d p 1 ⋯ d p n = N e − γ ( p ) / θ d p 1 ⋯ d p n {\displaystyle f_{\text{MJ}}(p,\theta )\,\mathrm {d} p_{1}\cdots \mathrm {d} p_{n}=N\,e^{-{\gamma (p)}/{\theta }}\,\mathrm {d} p_{1}\cdots \mathrm {d} p_{n}}

And the angular integration: d p 1 ⋯ d p n = B n p n − 1 d p = 1 2 B n ( m c ) n ( ( p m c ) 2 ) n 2 − 1 d ( p m c ) 2 , {\displaystyle \mathrm {d} p_{1}\cdots \mathrm {d} p_{n}=B_{n}p^{n-1}\,\mathrm {d} p={\frac {1}{2}}B_{n}\left(mc\right)^{n}\left(\left({\frac {p}{mc}}\right)^{2}\right)^{{\frac {n}{2}}-1}\,\mathrm {d} {\left({\frac {p}{mc}}\right)^{2}},}

Where B n = 2 π n / 2 Γ ( n / 2 ) {\displaystyle B_{n}={\frac {2\pi ^{n/2}}{\Gamma {\left(n/2\right)}}}} is the surface of the unit n-dimensional sphere. Then, using the identity γ 2 = 1 + ( p m c ) 2 {\textstyle \gamma ^{2}=1+\left({\frac {p}{mc}}\right)^{2}} one has: f MJ ( p ; θ ) d p 1 ⋯ d p n = N 2 B n ( m c ) n e − γ / θ ( γ 2 − 1 ) n 2 − 1 d ( γ 2 − 1 ) . {\displaystyle f_{\text{MJ}}(\mathbf {p} ;\theta )\,\mathrm {d} p_{1}\cdots \mathrm {d} p_{n}={\frac {N}{2}}B_{n}\left(mc\right)^{n}\,e^{-\gamma /\theta }\left(\gamma ^{2}-1\right)^{{\frac {n}{2}}-1}\,\mathrm {d} (\gamma ^{2}-1).} and 1 = ∫ − ∞ ∞ f MJ ( p ; θ ) d p 1 ⋯ d p n = N 2 B n ( m c ) n ∫ 1 ∞ e − γ θ ( γ 2 − 1 ) n 2 − 1 d ( γ 2 − 1 ) = N 2 B n ( n 2 ) − 1 ( m c ) n θ − 1 ∫ 1 ∞ e γ θ ( γ 2 − 1 ) n 2 d γ = N 2 B n ( n 2 ) − 1 ( m c ) n θ − 1 I n , {\displaystyle {\begin{aligned}1&=\int _{-\infty }^{\infty }f_{\text{MJ}}(\mathbf {p} ;\theta )\,\mathrm {d} p_{1}\cdots \mathrm {d} p_{n}\\[1ex]&={\frac {N}{2}}B_{n}\left(mc\right)^{n}\,\int _{1}^{\infty }e^{-{\frac {\gamma }{\theta }}}\left(\gamma ^{2}-1\right)^{{\frac {n}{2}}-1}\mathrm {d} (\gamma ^{2}-1)\\[1ex]&={\frac {N}{2}}B_{n}\left({\frac {n}{2}}\right)^{-1}\left(mc\right)^{n}\theta ^{-1}\,\int _{1}^{\infty }e^{\frac {\gamma }{\theta }}\left(\gamma ^{2}-1\right)^{\frac {n}{2}}\mathrm {d} \gamma \\[1ex]&={\frac {N}{2}}B_{n}\left({\frac {n}{2}}\right)^{-1}\left(mc\right)^{n}\theta ^{-1}\,I_{n},\end{aligned}}}

Where one has defined the integral:

I n ≡ ∫ 1 ∞ e − γ / θ ( γ 2 − 1 ) n / 2 d γ . {\displaystyle I_{n}\equiv \int _{1}^{\infty }e^{-\gamma /\theta }\left(\gamma ^{2}-1\right)^{n/2}\mathrm {d} \gamma .}

The Macdonald function (Modified Bessel function of the second kind) (Abramowitz and Stegun, 1972, p.376) is defined by:

K ν ⁡ ( z ) ≡ π 1 2 ( 1 2 z ) ν Γ ( ν + 1 2 ) ∫ 1 ∞ e − z γ ( γ 2 − 1 ) ν − 1 2 d γ {\displaystyle \operatorname {K} _{\nu }(z)\equiv {\frac {\pi ^{\frac {1}{2}}\left({\frac {1}{2}}z\right)^{\nu }}{\Gamma {\left(\nu +{\frac {1}{2}}\right)}}}\int _{1}^{\infty }e^{-z\gamma }\left(\gamma ^{2}-1\right)^{\nu -{\frac {1}{2}}}\,\mathrm {d} \gamma }

So that, by setting ν = n + 1 2 ,   z = 1 θ {\displaystyle \nu ={\frac {n+1}{2}},\ z={\frac {1}{\theta }}} one obtains:

I n = Γ ( n 2 + 1 ) π − 1 2 K n + 1 2 ⁡ ( 1 θ ) ( 2 θ ) n + 1 2 {\displaystyle I_{n}=\Gamma {\left({\frac {n}{2}}+1\right)}\pi ^{-{\frac {1}{2}}}\operatorname {K} _{\frac {n+1}{2}}{\!\!\left({\frac {1}{\theta }}\right)}\left(2\theta \right)^{\frac {n+1}{2}}}

Hence,

N − 1 = π n 2 Γ ( n 2 ) ( n 2 ) − 1 Γ ( n 2 + 1 ) π − 1 2 K n + 1 2 ⁡ ( 1 θ ) ( m c ) n ( 2 θ ) n + 1 2 = π n − 1 2 2 − n + 1 2 ( m c ) n θ n − 1 2 K n + 1 2 ⁡ ( 1 θ ) , {\displaystyle {\begin{aligned}N^{-1}&={\frac {\pi ^{\frac {n}{2}}}{\Gamma {\left({\frac {n}{2}}\right)}}}\left({\frac {n}{2}}\right)^{-1}\Gamma {\left({\frac {n}{2}}+1\right)}\pi ^{-{\frac {1}{2}}}\operatorname {K} _{\frac {n+1}{2}}{\!\!\left({\frac {1}{\theta }}\right)}\,\left(mc\right)^{n}\left(2\theta \right)^{\frac {n+1}{2}}\\[1ex]&=\pi ^{\frac {n-1}{2}}2^{-{\frac {n+1}{2}}}\left(mc\right)^{n}\,\theta ^{\frac {n-1}{2}}\operatorname {K} _{\frac {n+1}{2}}{\!\!\left({\frac {1}{\theta }}\right)},\end{aligned}}}

Or

N = π 1 − n 2 2 − n + 1 2 ( m c ) − n θ 1 − n 2 K n + 1 2 ⁡ ( 1 θ ) − 1 , {\displaystyle N=\pi ^{\frac {1-n}{2}}2^{-{\frac {n+1}{2}}}\left(mc\right)^{-n}\,\theta ^{\frac {1-n}{2}}\operatorname {K} _{\frac {n+1}{2}}{\!\!\left({\frac {1}{\theta }}\right)}^{-1},}

The inverse of the normalization constant gives the partition function Z ≡ 1 N {\displaystyle Z\equiv {\frac {1}{N}}} :

Z = π n − 1 2 2 − n + 1 2 ( m c ) n θ n − 1 2 K n + 1 2 ⁡ ( 1 θ ) , {\displaystyle Z=\pi ^{\frac {n-1}{2}}2^{-{\frac {n+1}{2}}}\left(mc\right)^{n}\,\theta ^{\frac {n-1}{2}}\operatorname {K} _{\frac {n+1}{2}}{\!\!\left({\frac {1}{\theta }}\right)},}

Therefore, the normalized distribution is:

f MJ ( p ; θ ) d p 1 ⋯ d p n = π 1 − n 2 2 − n + 1 2 ( m c ) − n θ 1 − n 2 e − γ ( p ) / θ K n + 1 2 ⁡ ( 1 θ ) d p 1 ⋯ d p n {\displaystyle f_{\text{MJ}}(p;\theta )\,\mathrm {d} p_{1}\cdots \mathrm {d} p_{n}=\pi ^{\frac {1-n}{2}}2^{-{\frac {n+1}{2}}}(mc)^{-n}\,\theta ^{\frac {1-n}{2}}{\frac {e^{-\gamma (p)/\theta }}{\operatorname {K} _{\frac {n+1}{2}}{\!\!\left({\frac {1}{\theta }}\right)}}}\,\mathrm {d} p_{1}\cdots \mathrm {d} p_{n}}

Or one may derive the normalised distribution in terms of:

f MJ ( γ ; θ ) d γ = π 1 2 2 1 − n 2 Γ ( n 2 ) θ 1 − n 2 e − γ / θ K n + 1 2 ⁡ ( 1 θ ) ( γ 2 − 1 ) n 2 − 1 γ d γ {\displaystyle f_{\text{MJ}}(\gamma ;\theta )\,\mathrm {d} \gamma ={\frac {\pi ^{\frac {1}{2}}2^{\frac {1-n}{2}}}{\Gamma {\left({\frac {n}{2}}\right)}}}\theta ^{\frac {1-n}{2}}{\frac {e^{-\gamma /\theta }}{\operatorname {K} _{\frac {n+1}{2}}{\!\!\left({\frac {1}{\theta }}\right)}}}\left(\gamma ^{2}-1\right)^{{\frac {n}{2}}-1}\gamma \,\mathrm {d} \gamma }

Note that θ {\displaystyle \theta } can be shown to coincide with the thermodynamic definition of temperature.

Also useful is the expression of the distribution in the velocity space.^[7] Given that d ( β γ ) d β = γ 3 {\displaystyle {\frac {\mathrm {d} (\beta \gamma )}{\mathrm {d} \beta }}=\gamma ^{3}} , one has:

d p 1 ⋯ d p n = p n − 1 d p d Ω n = ( m c ) n γ n − 1 β n − 1 d ( β γ ) d β d β d Ω n = ( m c ) n γ n + 2 β n − 1 d β d Ω n = ( m c ) n γ n + 2 d β 1 ⋯ d β n {\displaystyle {\begin{aligned}\mathrm {d} p_{1}\cdots \mathrm {d} p_{n}=p^{n-1}\,\mathrm {d} p\,\mathrm {d} \Omega _{n}&=\left(mc\right)^{n}\gamma ^{n-1}\beta ^{n-1}{\frac {\mathrm {d} (\beta \gamma )}{\mathrm {d} \beta }}\,\mathrm {d} \beta \,\mathrm {d} \Omega _{n}\\[1ex]&=\left(mc\right)^{n}\gamma ^{n+2}\beta ^{n-1}\,\mathrm {d} \beta \,\mathrm {d} \Omega _{n}\\[1ex]&=\left(mc\right)^{n}\gamma ^{n+2}\,\mathrm {d} \beta _{1}\cdots \mathrm {d} \beta _{n}\end{aligned}}}

Hence

f MJ ( β ; θ ) d β 1 ⋯ d β n = π 1 − n 2 2 − n + 1 2 θ 1 − n 2 e − γ ( β ) / θ K n + 1 2 ⁡ ( 1 θ ) γ ( β ) n + 2 d β 1 ⋯ d β n {\displaystyle f_{\text{MJ}}(\mathbf {\beta } ;\theta )\,\mathrm {d} \beta _{1}\cdots \mathrm {d} \beta _{n}=\pi ^{\frac {1-n}{2}}2^{-{\frac {n+1}{2}}}\,\theta ^{\frac {1-n}{2}}{\frac {e^{-\gamma (\beta )/\theta }}{\operatorname {K} _{\frac {n+1}{2}}{\!\!\left({\frac {1}{\theta }}\right)}}}\,\gamma (\beta )^{n+2}\,\mathrm {d} \beta _{1}\cdots \mathrm {d} \beta _{n}}

Take n = 3 {\displaystyle n=3} (the "classic case" in our world):

f MJ ( p ; θ ) d p 1 d p 2 d p 3 = e − γ ( p ) / θ θ K 2 ⁡ ( 1 / θ ) d p 1 d p 2 d p 3 4 π ( m c ) 3 , f MJ ( γ ; θ ) d γ = e − γ / θ ( γ 2 − 1 ) 1 / 2 θ K 2 ⁡ ( 1 / θ ) γ d γ , f MJ ( β ; θ ) d β 1 d β 2 d β 3 = e − γ ( β ) / θ γ ( β ) 5 θ K 2 ⁡ ( 1 / θ ) d β 1 d β 2 d β 3 4 π . {\displaystyle {\begin{aligned}f_{\text{MJ}}(p;\theta )\,\mathrm {d} p_{1}\,\mathrm {d} p_{2}\,\mathrm {d} p_{3}&={\frac {e^{-{\gamma (\mathbf {p} )/\theta }}}{\theta \,\operatorname {K} _{2}{\!\left(1/\theta \right)}}}\,{\frac {\mathrm {d} p_{1}\,\mathrm {d} p_{2}\,\mathrm {d} p_{3}}{4\pi \left(mc\right)^{3}}},\\[1ex]f_{\text{MJ}}(\gamma ;\theta )\,\mathrm {d} \gamma &={\frac {e^{-\gamma /\theta }\left(\gamma ^{2}-1\right)^{1/2}}{\theta \,\operatorname {K} _{2}{\!\left(1/\theta \right)}}}\,\gamma \,\mathrm {d} \gamma ,\\[1ex]f_{\text{MJ}}(\beta ;\theta )\,\mathrm {d} \beta _{1}\,\mathrm {d} \beta _{2}\,\mathrm {d} \beta _{3}&={\frac {e^{-\gamma (\beta )/\theta }\gamma (\beta )^{5}}{\theta \operatorname {K} _{2}{\!\left(1/\theta \right)}}}\,{\frac {\mathrm {d} \beta _{1}\,\mathrm {d} \beta _{2}\,\mathrm {d} \beta _{3}}{4\pi }}.\end{aligned}}}

Note that when the MB distribution clearly deviates from the MJ distribution of the same temperature and dimensionality, one can misinterpret and deduce a different MB distribution that will give a good approximation to the MJ distribution. This new MB distribution can be either:

• a convected MB distribution, that is, an MB distribution with the same dimensionality, but with different temperature T MB {\displaystyle T_{\text{MB}}} and bulk speed u b {\displaystyle \mathbf {u} _{b}} (or bulk energy E b ≡ 1 2 m ( u + u b ) 2 {\textstyle E_{b}\equiv {\frac {1}{2}}m\left(\mathbf {u} +\mathbf {u} _{b}\right)^{2}} )
• an MB distribution with the same bulk speed, but with different temperature T MB {\displaystyle T_{\text{MB}}} and degrees of freedom d MB {\displaystyle d_{\text{MB}}} . These two types of approximations are illustrated.

Other properties

The MJ probability density function is given by:

f MJ ( γ ) d γ = γ 2 β ( γ ) θ K 2 ⁡ ( 1 / θ ) e − γ / θ d γ {\displaystyle f_{\text{MJ}}(\gamma )\,\mathrm {d} \gamma ={\frac {\gamma ^{2}\,\beta (\gamma )}{\theta \operatorname {K} _{2}{\!\left(1/\theta \right)}}}\,e^{-{\gamma }/{\theta }}\,\mathrm {d} \gamma }

This means that a relativistic non-quantum particle with parameter θ {\displaystyle \theta } has a probability of f MJ ( γ ) d γ {\displaystyle f_{\text{MJ}}(\gamma )\,\mathrm {d} \gamma } of having its Lorentz factor in the interval [ γ , γ + d γ ] {\displaystyle [\gamma ,\gamma +\mathrm {d} \gamma ]} .

References

 This article incorporates text by George Livadiotis available under the CC BY 3.0 license.