# 配分函数

In physics, a partition function describes the statistical properties of a system in thermodynamic equilibrium.[citation needed] Partition functions are functions of the thermodynamic state variables, such as the temperature and volume. Most of the aggregate thermodynamic variables of the system, such as the total energy, free energy, entropy, and pressure, can be expressed in terms of the partition function or its derivatives. The partition function is dimensionless, it is a pure number.

In physics, a partition function describes the statistical properties of a system in thermodynamic equilibrium. Partition functions are functions of the thermodynamic state variables, such as the temperature and volume. Most of the aggregate thermodynamic variables of the system, such as the total energy, free energy, entropy, and pressure, can be expressed in terms of the partition function or its derivatives. The partition function is dimensionless, it is a pure number.

Each partition function is constructed to represent a particular statistical ensemble (which, in turn, corresponds to a particular free energy). The most common statistical ensembles have named partition functions. The canonical partition function applies to a canonical ensemble, in which the system is allowed to exchange heat with the environment at fixed temperature, volume, and number of particles. The grand canonical partition function applies to a grand canonical ensemble, in which the system can exchange both heat and particles with the environment, at fixed temperature, volume, and chemical potential. Other types of partition functions can be defined for different circumstances; see partition function (mathematics) for generalizations. The partition function has many physical meanings, as discussed in Meaning and significance.

Each partition function is constructed to represent a particular statistical ensemble (which, in turn, corresponds to a particular free energy). The most common statistical ensembles have named partition functions. The canonical partition function applies to a canonical ensemble, in which the system is allowed to exchange heat with the environment at fixed temperature, volume, and number of particles. The grand canonical partition function applies to a grand canonical ensemble, in which the system can exchange both heat and particles with the environment, at fixed temperature, volume, and chemical potential. Other types of partition functions can be defined for different circumstances; see partition function (mathematics) for generalizations. The partition function has many physical meanings, as discussed in Meaning and significance.

## Canonical partition function

### Definition

Initially, let us assume that a thermodynamically large system is in thermal contact with the environment, with a temperature T, and both the volume of the system and the number of constituent particles are fixed. A collection of this kind of systems comprises an ensemble called a canonical ensemble. The appropriate mathematical expression for the canonical partition function depends on the degrees of freedom of the system, whether the context is classical mechanics or quantum mechanics, and whether the spectrum of states is discrete or continuous.[citation needed]

Initially, let us assume that a thermodynamically large system is in thermal contact with the environment, with a temperature T, and both the volume of the system and the number of constituent particles are fixed. A collection of this kind of systems comprises an ensemble called a canonical ensemble. The appropriate mathematical expression for the canonical partition function depends on the degrees of freedom of the system, whether the context is classical mechanics or quantum mechanics, and whether the spectrum of states is discrete or continuous.

Classical discrete system

Classical discrete system

For a canonical ensemble that is classical and discrete, the canonical partition function is defined as

For a canonical ensemble that is classical and discrete, the canonical partition function is defined as

$\displaystyle{ Z = \sum_{i} \mathrm{e}^{-\beta E_i}, }$
$\displaystyle{ Z = \sum_{i} \mathrm{e}^{-\beta E_i}, }$


[数学] z = sum { i } mathrm { e } ^ {-beta e _ i } ，[数学]

where

where

$\displaystyle{ i }$ is the index for the microstates of the system;
$\displaystyle{ i }$ is the index for the microstates of the system;


$\displaystyle{ \mathrm{e} }$ is Euler's number;
$\displaystyle{ \mathrm{e} }$ is Euler's number;


$\displaystyle{ \beta }$ is the thermodynamic beta, defined as $\displaystyle{ \tfrac{1}{k_\text{B} T} }$;
$\displaystyle{ \beta }$ is the thermodynamic beta, defined as $\displaystyle{ \tfrac{1}{k_\text{B} T} }$;


$\displaystyle{ E_i }$ is the total energy of the system in the respective microstate.
$\displaystyle{ E_i }$ is the total energy of the system in the respective microstate.


The exponential factor $\displaystyle{ \mathrm{e}^{-\beta E_i} }$ is otherwise known as the Boltzmann factor.

The exponential factor $\displaystyle{ \mathrm{e}^{-\beta E_i} }$ is otherwise known as the Boltzmann factor.

{ | class = “ toccolours collable collapsed” width = “60% ” style = “ text-align: left”

|}

Classical continuous system

Classical continuous system

In classical mechanics, the position and momentum variables of a particle can vary continuously, so the set of microstates is actually uncountable. In classical statistical mechanics, it is rather inaccurate to express the partition function as a sum of discrete terms. In this case we must describe the partition function using an integral rather than a sum. For a canonical ensemble that is classical and continuous, the canonical partition function is defined as

In classical mechanics, the position and momentum variables of a particle can vary continuously, so the set of microstates is actually uncountable. In classical statistical mechanics, it is rather inaccurate to express the partition function as a sum of discrete terms. In this case we must describe the partition function using an integral rather than a sum. For a canonical ensemble that is classical and continuous, the canonical partition function is defined as

$\displaystyle{ Z = \frac{1}{h^3} \int \mathrm{e}^{-\beta H(q, p)} \, \mathrm{d}^3 q \, \mathrm{d}^3 p, }$
$\displaystyle{ Z = \frac{1}{h^3} \int \mathrm{e}^{-\beta H(q, p)} \, \mathrm{d}^3 q \, \mathrm{d}^3 p, }$


< math > z = frac {1}{ h ^ 3} int mathrm { e } ^ {-beta h (q，p)} ，mathrm { d } ^ 3 q，mathrm { d } ^ 3 p，</math >

where

where

$\displaystyle{ h }$ is the Planck constant;
$\displaystyle{ h }$ is the Planck constant;


$\displaystyle{ \beta }$ is the thermodynamic beta, defined as $\displaystyle{ \tfrac{1}{k_\text{B} T} }$;
$\displaystyle{ \beta }$ is the thermodynamic beta, defined as $\displaystyle{ \tfrac{1}{k_\text{B} T} }$;


$\displaystyle{ H(q, p) }$ is the Hamiltonian of the system;
$\displaystyle{ H(q, p) }$ is the Hamiltonian of the system;


H (q，p) </math > 是系统的哈密顿函数;

$\displaystyle{ q }$ is the canonical position;
$\displaystyle{ q }$ is the canonical position;


Q </math > 是典型的位置

$\displaystyle{ p }$ is the canonical momentum.
$\displaystyle{ p }$ is the canonical momentum.


To make it into a dimensionless quantity, we must divide it by h, which is some quantity with units of action (usually taken to be Planck's constant).

To make it into a dimensionless quantity, we must divide it by h, which is some quantity with units of action (usually taken to be Planck's constant).

Classical continuous system (multiple identical particles)

Classical continuous system (multiple identical particles)

For a gas of $\displaystyle{ N }$ identical classical particles in three dimensions, the partition function is

For a gas of $\displaystyle{ N }$ identical classical particles in three dimensions, the partition function is

$\displaystyle{ Z=\frac{1}{N!h^{3N}} \int \, \exp \left(-\beta \sum_{i=1}^N H(\textbf q_i, \textbf p_i) \right) \; \mathrm{d}^3 q_1 \cdots \mathrm{d}^3 q_N \, \mathrm{d}^3 p_1 \cdots \mathrm{d}^3 p_N }$
$\displaystyle{ Z=\frac{1}{N!h^{3N}} \int \, \exp \left(-\beta \sum_{i=1}^N H(\textbf q_i, \textbf p_i) \right) \; \mathrm{d}^3 q_1 \cdots \mathrm{d}^3 q_N \, \mathrm{d}^3 p_1 \cdots \mathrm{d}^3 p_N }$


[数学] z = frac {1}{ n! h ^ {3N } int，exp left (- beta sum { i = 1} ^ n h (textbf q _ i，textbf p _ i) right) ; mathrm { d } ^ 3 q _ 1 cdots mathrm { d } ^ 3 q _ n，mathrm { d } ^ 3 p _ 1 cdots mathrm { d } ^ 3 p _ n </math >

where

where

$\displaystyle{ h }$ is the Planck constant;
$\displaystyle{ h }$ is the Planck constant;


$\displaystyle{ \beta }$ is the thermodynamic beta, defined as $\displaystyle{ \tfrac{1}{k_\text{B} T} }$;
$\displaystyle{ \beta }$ is the thermodynamic beta, defined as $\displaystyle{ \tfrac{1}{k_\text{B} T} }$;


$\displaystyle{ i }$ is the index for the particles of the system;
$\displaystyle{ i }$ is the index for the particles of the system;


$\displaystyle{ H }$ is the Hamiltonian of a respective particle;
$\displaystyle{ H }$ is the Hamiltonian of a respective particle;


$\displaystyle{ q_i }$ is the canonical position of the respective particle;
$\displaystyle{ q_i }$ is the canonical position of the respective particle;


$\displaystyle{ p_i }$ is the canonical momentum of the respective particle;
$\displaystyle{ p_i }$ is the canonical momentum of the respective particle;


$\displaystyle{ \mathrm{d}^3 }$ is shorthand notation to indicate that $\displaystyle{ q_i }$ and $\displaystyle{ p_i }$ are vectors in three-dimensional space.
$\displaystyle{ \mathrm{d}^3 }$ is shorthand notation to indicate that $\displaystyle{ q_i }$ and $\displaystyle{ p_i }$ are vectors in three-dimensional space.


The reason for the factorial factor N! is discussed below. The extra constant factor introduced in the denominator was introduced because, unlike the discrete form, the continuous form shown above is not dimensionless. As stated in the previous section, to make it into a dimensionless quantity, we must divide it by h3N (where h is usually taken to be Planck's constant).

The reason for the factorial factor N! is discussed below. The extra constant factor introduced in the denominator was introduced because, unlike the discrete form, the continuous form shown above is not dimensionless. As stated in the previous section, to make it into a dimensionless quantity, we must divide it by h3N (where h is usually taken to be Planck's constant).

Quantum mechanical discrete system

Quantum mechanical discrete system

For a canonical ensemble that is quantum mechanical and discrete, the canonical partition function is defined as the trace of the Boltzmann factor:

For a canonical ensemble that is quantum mechanical and discrete, the canonical partition function is defined as the trace of the Boltzmann factor:

$\displaystyle{ Z = \operatorname{tr} ( \mathrm{e}^{-\beta \hat{H}} ), }$
$\displaystyle{ Z = \operatorname{tr} ( \mathrm{e}^{-\beta \hat{H}} ), }$


[ math > z = operatorname { tr }(mathrm { e } ^ {-beta hat { h }) ，</math >

where:

where:

$\displaystyle{ \operatorname{tr} ( \circ ) }$ is the trace of a matrix;
$\displaystyle{ \operatorname{tr} ( \circ ) }$ is the trace of a matrix;


$\displaystyle{ \beta }$ is the thermodynamic beta, defined as $\displaystyle{ \tfrac{1}{k_\text{B} T} }$;
$\displaystyle{ \beta }$ is the thermodynamic beta, defined as $\displaystyle{ \tfrac{1}{k_\text{B} T} }$;


$\displaystyle{ \hat{H} }$ is the Hamiltonian operator.
$\displaystyle{ \hat{H} }$ is the Hamiltonian operator.


The dimension of $\displaystyle{ \mathrm{e}^{-\beta \hat{H}} }$ is the number of energy eigenstates of the system.

The dimension of $\displaystyle{ \mathrm{e}^{-\beta \hat{H}} }$ is the number of energy eigenstates of the system.

Quantum mechanical continuous system

Quantum mechanical continuous system

For a canonical ensemble that is quantum mechanical and continuous, the canonical partition function is defined as

For a canonical ensemble that is quantum mechanical and continuous, the canonical partition function is defined as

$\displaystyle{ Z = \frac{1}{h} \int \langle q, p | \mathrm{e}^{-\beta \hat{H}} | q, p \rangle \, \mathrm{d} q \, \mathrm{d} p, }$
$\displaystyle{ Z = \frac{1}{h} \int \langle q, p | \mathrm{e}^{-\beta \hat{H}} | q, p \rangle \, \mathrm{d} q \, \mathrm{d} p, }$


1}{ h } int langle q，p | mathrm { e } ^ {-beta hat { h } | q，p rangle，mathrm { d } q，mathrm { d } p，</math >

where:

where:

$\displaystyle{ h }$ is the Planck constant;
$\displaystyle{ h }$ is the Planck constant;


$\displaystyle{ \beta }$ is the thermodynamic beta, defined as $\displaystyle{ \tfrac{1}{k_\text{B} T} }$;
$\displaystyle{ \beta }$ is the thermodynamic beta, defined as $\displaystyle{ \tfrac{1}{k_\text{B} T} }$;


$\displaystyle{ \hat{H} }$ is the Hamiltonian operator;
$\displaystyle{ \hat{H} }$ is the Hamiltonian operator;


$\displaystyle{ q }$ is the canonical position;
$\displaystyle{ q }$ is the canonical position;


Q </math > 是典型的位置

$\displaystyle{ p }$ is the canonical momentum.
$\displaystyle{ p }$ is the canonical momentum.


In systems with multiple quantum states s sharing the same energy Es, it is said that the energy levels of the system are degenerate. In the case of degenerate energy levels, we can write the partition function in terms of the contribution from energy levels (indexed by j) as follows:

In systems with multiple quantum states s sharing the same energy Es, it is said that the energy levels of the system are degenerate. In the case of degenerate energy levels, we can write the partition function in terms of the contribution from energy levels (indexed by j) as follows:

$\displaystyle{ Z = \sum_j g_j \cdot \mathrm{e}^{-\beta E_j}, }$
$\displaystyle{ Z = \sum_j g_j \cdot \mathrm{e}^{-\beta E_j}, }$


[数学，数学]

where gj is the degeneracy factor, or number of quantum states s that have the same energy level defined by Ej = Es.

where gj is the degeneracy factor, or number of quantum states s that have the same energy level defined by Ej = Es.

The above treatment applies to quantum statistical mechanics, where a physical system inside a finite-sized box will typically have a discrete set of energy eigenstates, which we can use as the states s above. In quantum mechanics, the partition function can be more formally written as a trace over the state space (which is independent of the choice of basis):

The above treatment applies to quantum statistical mechanics, where a physical system inside a finite-sized box will typically have a discrete set of energy eigenstates, which we can use as the states s above. In quantum mechanics, the partition function can be more formally written as a trace over the state space (which is independent of the choice of basis):

$\displaystyle{ Z = \operatorname{tr} ( \mathrm{e}^{-\beta \hat{H}} ), }$
$\displaystyle{ Z = \operatorname{tr} ( \mathrm{e}^{-\beta \hat{H}} ), }$


[ math > z = operatorname { tr }(mathrm { e } ^ {-beta hat { h }) ，</math >

where Ĥ is the quantum Hamiltonian operator. The exponential of an operator can be defined using the exponential power series.

where Ĥ is the quantum Hamiltonian operator. The exponential of an operator can be defined using the exponential power series.

The classical form of Z is recovered when the trace is expressed in terms of coherent states[1]

are regarded as negligible. Formally, using bra–ket notation, one inserts under the trace for each degree of freedom the identity:

and when quantum-mechanical uncertainties in the position and momentum of a particle

$\displaystyle{ 《数学》 are regarded as negligible. Formally, using [[bra–ket notation]], one inserts under the trace for each degree of freedom the identity: \boldsymbol{1} = \int |x, p\rangle \langle x,p| \frac{dx \,dp}{h}, 1} = int | x，p rangle langle x，p | frac { dx，dp }{ h } , :\lt math\gt }$

\boldsymbol{1} = \int |x, p\rangle \langle x,p| \frac{dx \,dp}{h},


where x, p is a normalised Gaussian wavepacket centered at

[/itex]

position x and momentum p. Thus

where |x, p模板:Rangle is a normalised Gaussian wavepacket centered at

$\displaystyle{ 《数学》 position ''x'' and momentum ''p''. Thus Z = \int \operatorname{tr} \left( \mathrm{e}^{-\beta\hat{H}} |x, p\rangle \langle x, p| \right) \frac{dx \,dp}{h} Z = int operatorname { tr } left (mathrm { e } ^ {-beta hat { h } | x，p rangle langle x，p | right) frac { dx，dp }{ h } :\lt math\gt = \int \langle x,p| \mathrm{e}^{-\beta\hat{H}} |x, p\rangle \frac{dx \,dp}{h}. = int langle x，p | mathrm { e } ^ {-beta hat { h } | x，p rangle frac { dx，dp }{ h }. Z = \int \operatorname{tr} \left( \mathrm{e}^{-\beta\hat{H}} |x, p\rangle \langle x, p| \right) \frac{dx \,dp}{h} }$

  = \int \langle x,p| \mathrm{e}^{-\beta\hat{H}} |x, p\rangle \frac{dx \,dp}{h}.


A coherent state is an approximate eigenstate of both operators $\displaystyle{ \hat{x} }$ and $\displaystyle{ \hat{p} }$, hence also of the Hamiltonian Ĥ, with errors of the size of the uncertainties. If Δx and Δp can be regarded as zero, the action of Ĥ reduces to multiplication by the classical Hamiltonian, and Z reduces to the classical configuration integral.

[/itex]

A coherent state is an approximate eigenstate of both operators $\displaystyle{ \hat{x} }$ and $\displaystyle{ \hat{p} }$, hence also of the Hamiltonian Ĥ, with errors of the size of the uncertainties. If Δx and Δp can be regarded as zero, the action of Ĥ reduces to multiplication by the classical Hamiltonian, and Z reduces to the classical configuration integral.

### Connection to probability theory

For simplicity, we will use the discrete form of the partition function in this section. Our results will apply equally well to the continuous form.

For simplicity, we will use the discrete form of the partition function in this section. Our results will apply equally well to the continuous form.

Consider a system S embedded into a heat bath B. Let the total energy of both systems be E. Let pi denote the probability that the system S is in a particular microstate, i, with energy Ei. According to the fundamental postulate of statistical mechanics (which states that all attainable microstates of a system are equally probable), the probability pi will be proportional to the number of microstates of the total closed system (S, B) in which S is in microstate i with energy Ei. Equivalently, pi will be proportional to the number of microstates of the heat bath B with energy E − Ei:

Consider a system S embedded into a heat bath B. Let the total energy of both systems be E. Let pi denote the probability that the system S is in a particular microstate, i, with energy Ei. According to the fundamental postulate of statistical mechanics (which states that all attainable microstates of a system are equally probable), the probability pi will be proportional to the number of microstates of the total closed system (S, B) in which S is in microstate i with energy Ei. Equivalently, pi will be proportional to the number of microstates of the heat bath B with energy EEi:

$\displaystyle{ 《数学》 p_i = \frac{\Omega_B(E - E_i)}{\Omega_{(S,B)}(E)}. P _ i = frac { Omega _ b (e-e _ i)}{ Omega _ {(s，b)}(e)}. :\lt math\gt }$

p_i = \frac{\Omega_B(E - E_i)}{\Omega_{(S,B)}(E)}.


[/itex]

Assuming that the heat bath's internal energy is much larger than the energy of S (E ≫ Ei), we can Taylor-expand $\displaystyle{ \Omega_B }$ to first order in Ei and use the thermodynamic relation $\displaystyle{ \partial S_B/\partial E = 1/T }$, where here $\displaystyle{ S_B }$, $\displaystyle{ T }$ are the entropy and temperature of the bath respectively:

Assuming that the heat bath's internal energy is much larger than the energy of S (EEi), we can Taylor-expand $\displaystyle{ \Omega_B }$ to first order in Ei and use the thermodynamic relation $\displaystyle{ \partial S_B/\partial E = 1/T }$, where here $\displaystyle{ S_B }$, $\displaystyle{ T }$ are the entropy and temperature of the bath respectively:

\displaystyle{ 《数学》 \begin{align} 开始{ align } :\lt math\gt k \ln p_i &= k \ln \Omega_B(E - E_i) - k \ln \Omega_{(S,B)}(E) \\[5pt] K ln p _ i & = k ln Omega _ b (e-e _ i)-k ln Omega _ (s，b)}(e)[5 pt ] \begin{align} &\approx -\frac{\partial\big(k \ln \Omega_B(E)\big)}{\partial E} E_i + k \ln\Omega_B(E) - k \ln \Omega_{(S,B)}(E) 大约-frac { partial big (k ln Omega _ b (e) big)}{ partial e } e _ i + k ln Omega _ b (e)-k ln Omega _ {(s，b)}(e)) k \ln p_i &= k \ln \Omega_B(E - E_i) - k \ln \Omega_{(S,B)}(E) \\[5pt] \\[5pt] [5 pt ] &\approx -\frac{\partial\big(k \ln \Omega_B(E)\big)}{\partial E} E_i + k \ln\Omega_B(E) - k \ln \Omega_{(S,B)}(E) &\approx -\frac{\partial S_B}{\partial E} E_i + k \ln \frac{\Omega_B(E)}{\Omega_{(S,B)}(E)} \\[5pt] 大约-frac { partial s _ b }{ partial e } e _ i + k ln frac { Omega _ b (e)}{ Omega _ {(s，b)}(e)}[5 pt ] \\[5pt] &\approx -\frac{E_i}{T} + k \ln \frac{\Omega_B(E)}{\Omega_{(S,B)}(E)} 约-frac { e _ i }{ t } + k ln frac { Omega _ b (e)}{ Omega _ {(s，b)}(e)} &\approx -\frac{\partial S_B}{\partial E} E_i + k \ln \frac{\Omega_B(E)}{\Omega_{(S,B)}(E)} \\[5pt] \end{align} 结束{ align } &\approx -\frac{E_i}{T} + k \ln \frac{\Omega_B(E)}{\Omega_{(S,B)}(E)} }

\end{align}

[/itex]

Thus

$\displaystyle{ 《数学》 Thus p_i \propto e^{-E_i/(kT)} = e^{-\beta E_i}. P _ i propto e ^ {-e _ i/(kT)} = e ^ {-beta e _ i }. :\lt math\gt }$

p_i \propto e^{-E_i/(kT)} = e^{-\beta E_i}.


[/itex]

Since the total probability to find the system in some microstate (the sum of all pi) must be equal to 1, we know that the constant of proportionality must be the normalization constant, and so, we can define the partition function to be this constant:

Since the total probability to find the system in some microstate (the sum of all pi) must be equal to 1, we know that the constant of proportionality must be the normalization constant, and so, we can define the partition function to be this constant:

$\displaystyle{ 《数学》 Z = \sum_i e^{-\beta E_i} = \frac{\Omega_{(S,B)}(E)}{\Omega_B(E)}. Z = sum _ i e ^ {-beta e _ i } = frac { Omega _ {(s，b)}(e)}{ Omega _ b (e)}. :\lt math\gt }$

Z =  \sum_i e^{-\beta E_i} = \frac{\Omega_{(S,B)}(E)}{\Omega_B(E)}.


[/itex]

### Calculating the thermodynamic total energy

In order to demonstrate the usefulness of the partition function, let us calculate the thermodynamic value of the total energy. This is simply the expected value, or ensemble average for the energy, which is the sum of the microstate energies weighted by their probabilities:

In order to demonstrate the usefulness of the partition function, let us calculate the thermodynamic value of the total energy. This is simply the expected value, or ensemble average for the energy, which is the sum of the microstate energies weighted by their probabilities:

$\displaystyle{ \langle E \rangle = \sum_s E_s P_s = \frac{1}{Z} \sum_s E_s [数学]长角 e rangle = sum _ s e _ s p _ s = frac {1}{ z } sum _ s e _ s e^{- \beta E_s} = - \frac{1}{Z} \frac{\partial}{\partial \beta} E ^ {-beta e _ s } =-frac {1}{ z } frac { partial beta } : \lt math\gt \langle E \rangle = \sum_s E_s P_s = \frac{1}{Z} \sum_s E_s Z(\beta, E_1, E_2, \cdots) = - \frac{\partial \ln Z}{\partial \beta} Z (beta，e_1，e_2，cdots) =-frac { partial ln z }{ partial beta } e^{- \beta E_s} = - \frac{1}{Z} \frac{\partial}{\partial \beta} }$


Z(\beta, E_1, E_2, \cdots) = - \frac{\partial \ln Z}{\partial \beta}

[/itex]

or, equivalently,

or, equivalently,

$\displaystyle{ \langle E\rangle = k_B T^2 \frac{\partial \ln Z}{\partial T}. }$


[数学]长角 e rangle = k _ b t ^ 2 frac { partial ln z }{ partial t }

$\displaystyle{ \langle E\rangle = k_B T^2 \frac{\partial \ln Z}{\partial T}. }$

Incidentally, one should note that if the microstate energies depend on a parameter λ in the manner

Incidentally, one should note that if the microstate energies depend on a parameter λ in the manner

$\displaystyle{ E_s = E_s^{(0)} + \lambda A_s \qquad \mbox{for all}\; s }$


[所有} ; s </math >

$\displaystyle{ E_s = E_s^{(0)} + \lambda A_s \qquad \mbox{for all}\; s }$

then the expected value of A is

then the expected value of A is

$\displaystyle{ \langle A\rangle = \sum_s A_s P_s = -\frac{1}{\beta} 1. a rangle = sum _ s a _ s p _ s =-frac {1}{ beta } \frac{\partial}{\partial\lambda} \ln Z(\beta,\lambda). }$


{ partial }{ partial lambda } ln z (beta，lambda) . </math >

$\displaystyle{ \langle A\rangle = \sum_s A_s P_s = -\frac{1}{\beta} \frac{\partial}{\partial\lambda} \ln Z(\beta,\lambda). }$

This provides us with a method for calculating the expected values of many microscopic quantities. We add the quantity artificially to the microstate energies (or, in the language of quantum mechanics, to the Hamiltonian), calculate the new partition function and expected value, and then set λ to zero in the final expression. This is analogous to the source field method used in the path integral formulation of quantum field theory.

This provides us with a method for calculating the expected values of many microscopic quantities. We add the quantity artificially to the microstate energies (or, in the language of quantum mechanics, to the Hamiltonian), calculate the new partition function and expected value, and then set λ to zero in the final expression. This is analogous to the source field method used in the path integral formulation of quantum field theory.[citation needed]

### Relation to thermodynamic variables

In this section, we will state the relationships between the partition function and the various thermodynamic parameters of the system. These results can be derived using the method of the previous section and the various thermodynamic relations.

In this section, we will state the relationships between the partition function and the various thermodynamic parameters of the system. These results can be derived using the method of the previous section and the various thermodynamic relations.

As we have already seen, the thermodynamic energy is

As we have already seen, the thermodynamic energy is

$\displaystyle{ \langle E \rangle = - \frac{\partial \ln Z}{\partial \beta}. }$


[数学][数学]

$\displaystyle{ \langle E \rangle = - \frac{\partial \ln Z}{\partial \beta}. }$

The variance in the energy (or "energy fluctuation") is

The variance in the energy (or "energy fluctuation") is

$\displaystyle{ \langle (\Delta E)^2 \rangle \equiv \langle (E - \langle 2rangle equiv langle (e-langle)2 rangle equiv langle E\rangle)^2 \rangle = \frac{\partial^2 \ln Z}{\partial \beta^2}. }$


2 rangle = frac { partial ^ 2 ln z }{ partial beta ^ 2} . </math >

$\displaystyle{ \langle (\Delta E)^2 \rangle \equiv \langle (E - \langle E\rangle)^2 \rangle = \frac{\partial^2 \ln Z}{\partial \beta^2}. }$

The heat capacity is

The heat capacity is

$\displaystyle{ C_v = \frac{\partial \langle E\rangle}{\partial T} = \frac{1}{k_B T^2} \langle (\Delta E)^2 \rangle. }$


[ math > c _ v = frac { partial langle e rangle }{ partial t } = frac {1}{ k _ b t ^ 2} langle (Delta e) ^ 2 rangle

$\displaystyle{ C_v = \frac{\partial \langle E\rangle}{\partial T} = \frac{1}{k_B T^2} \langle (\Delta E)^2 \rangle. }$

In general, consider the extensive variable X and intensive variable Y where X and Y form a pair of conjugate variables. In ensembles where Y is fixed (and X is allowed to fluctuate), then the average value of X will be:

In general, consider the extensive variable X and intensive variable Y where X and Y form a pair of conjugate variables. In ensembles where Y is fixed (and X is allowed to fluctuate), then the average value of X will be:

$\displaystyle{ \langle X \rangle = \pm \frac{\partial \ln Z}{\partial \beta Y}. }$


[数学][数学]

$\displaystyle{ \langle X \rangle = \pm \frac{\partial \ln Z}{\partial \beta Y}. }$

The sign will depend on the specific definitions of the variables X and Y. An example would be X = volume and Y = pressure. Additionally, the variance in X will be

The sign will depend on the specific definitions of the variables X and Y. An example would be X = volume and Y = pressure. Additionally, the variance in X will be

$\displaystyle{ \langle (\Delta X)^2 \rangle \equiv \langle (X - \langle 2rangle equiv langle (x-langle X\rangle)^2 \rangle = \frac{\partial \langle X \rangle}{\partial \beta Y} = \frac{\partial^2 \ln Z}{\partial (\beta Y)^2}. }$


2 rangle = frac { partial angle x rangle }{ partial beta y } = frac { partial ^ 2 ln z }{ partial (beta y) ^ 2} . </math >

$\displaystyle{ \langle (\Delta X)^2 \rangle \equiv \langle (X - \langle X\rangle)^2 \rangle = \frac{\partial \langle X \rangle}{\partial \beta Y} = \frac{\partial^2 \ln Z}{\partial (\beta Y)^2}. }$

In the special case of entropy, entropy is given by

In the special case of entropy, entropy is given by

$\displaystyle{ S \equiv -k_B\sum_s P_s\ln P_s= k_B (\ln Z + \beta \langle E\rangle)=\frac{\partial}{\partial T}(k_B T \ln Z) =-\frac{\partial A}{\partial T} }$


= frac { partial }{ t }(k _ b t ln z) =-frac { partial a }{ partial t } </math >

$\displaystyle{ S \equiv -k_B\sum_s P_s\ln P_s= k_B (\ln Z + \beta \langle E\rangle)=\frac{\partial}{\partial T}(k_B T \ln Z) =-\frac{\partial A}{\partial T} }$

where A is the Helmholtz free energy defined as A = U − TS, where U = E is the total energy and S is the entropy, so that

where A is the Helmholtz free energy defined as A = UTS, where U = 模板:LangleE模板:Rangle is the total energy and S is the entropy, so that

$\displaystyle{ A = \langle E\rangle -TS= - k_B T \ln Z. }$


A = langle e rangle-TS =-k _ b t ln z

$\displaystyle{ A = \langle E\rangle -TS= - k_B T \ln Z. }$

### Partition functions of subsystems

Suppose a system is subdivided into N sub-systems with negligible interaction energy, that is, we can assume the particles are essentially non-interacting. If the partition functions of the sub-systems are ζ1, ζ2, ..., ζN, then the partition function of the entire system is the product of the individual partition functions:

Suppose a system is subdivided into N sub-systems with negligible interaction energy, that is, we can assume the particles are essentially non-interacting. If the partition functions of the sub-systems are ζ1, ζ2, ..., ζN, then the partition function of the entire system is the product of the individual partition functions:

$\displaystyle{ Z =\prod_{j=1}^{N} \zeta_j. }$


[数学] z = prod { j = 1} ^ { n } zeta _ j

$\displaystyle{ Z =\prod_{j=1}^{N} \zeta_j. }$

If the sub-systems have the same physical properties, then their partition functions are equal, ζ1 = ζ2 = ... = ζ, in which case

If the sub-systems have the same physical properties, then their partition functions are equal, ζ1 = ζ2 = ... = ζ, in which case

$\displaystyle{ Z = \zeta^N. }$


Z = zeta ^ n

$\displaystyle{ Z = \zeta^N. }$

However, there is a well-known exception to this rule. If the sub-systems are actually identical particles, in the quantum mechanical sense that they are impossible to distinguish even in principle, the total partition function must be divided by a N! (N factorial):

However, there is a well-known exception to this rule. If the sub-systems are actually identical particles, in the quantum mechanical sense that they are impossible to distinguish even in principle, the total partition function must be divided by a N! (N factorial):

$\displaystyle{ Z = \frac{\zeta^N}{N!}. }$


$\displaystyle{ Z = \frac{\zeta^N}{N!}. }$

This is to ensure that we do not "over-count" the number of microstates. While this may seem like a strange requirement, it is actually necessary to preserve the existence of a thermodynamic limit for such systems. This is known as the Gibbs paradox.

This is to ensure that we do not "over-count" the number of microstates. While this may seem like a strange requirement, it is actually necessary to preserve the existence of a thermodynamic limit for such systems. This is known as the Gibbs paradox.

### Meaning and significance

It may not be obvious why the partition function, as we have defined it above, is an important quantity. First, consider what goes into it. The partition function is a function of the temperature T and the microstate energies E1, E2, E3, etc. The microstate energies are determined by other thermodynamic variables, such as the number of particles and the volume, as well as microscopic quantities like the mass of the constituent particles. This dependence on microscopic variables is the central point of statistical mechanics. With a model of the microscopic constituents of a system, one can calculate the microstate energies, and thus the partition function, which will then allow us to calculate all the other thermodynamic properties of the system.

It may not be obvious why the partition function, as we have defined it above, is an important quantity. First, consider what goes into it. The partition function is a function of the temperature T and the microstate energies E1, E2, E3, etc. The microstate energies are determined by other thermodynamic variables, such as the number of particles and the volume, as well as microscopic quantities like the mass of the constituent particles. This dependence on microscopic variables is the central point of statistical mechanics. With a model of the microscopic constituents of a system, one can calculate the microstate energies, and thus the partition function, which will then allow us to calculate all the other thermodynamic properties of the system.

The partition function can be related to thermodynamic properties because it has a very important statistical meaning. The probability Ps that the system occupies microstate s is

The partition function can be related to thermodynamic properties because it has a very important statistical meaning. The probability Ps that the system occupies microstate s is

$\displaystyle{ P_s = \frac{1}{Z} \mathrm{e}^{- \beta E_s}. }$


< math > p _ s = frac {1}{ z } mathrm { e } ^ {-beta e _ s }.数学

$\displaystyle{ P_s = \frac{1}{Z} \mathrm{e}^{- \beta E_s}. }$

Thus, as shown above, the partition function plays the role of a normalizing constant (note that it does not depend on s), ensuring that the probabilities sum up to one:

Thus, as shown above, the partition function plays the role of a normalizing constant (note that it does not depend on s), ensuring that the probabilities sum up to one:

$\displaystyle{ \sum_s P_s = \frac{1}{Z} \sum_s \mathrm{e}^{- \beta E_s} = \frac{1}{Z} Z 1}{ z } sum s mathrm { e } ^ {-beta e _ s } = frac {1}{ z } z = 1. }$


= 1.数学

$\displaystyle{ \sum_s P_s = \frac{1}{Z} \sum_s \mathrm{e}^{- \beta E_s} = \frac{1}{Z} Z = 1. }$

This is the reason for calling Z the "partition function": it encodes how the probabilities are partitioned among the different microstates, based on their individual energies. The letter Z stands for the German word Zustandssumme, "sum over states". The usefulness of the partition function stems from the fact that it can be used to relate macroscopic thermodynamic quantities to the microscopic details of a system through the derivatives of its partition function. Finding the partition function is also equivalent to performing a Laplace transform of the density of states function from the energy domain to the β domain, and the inverse Laplace transform of the partition function reclaims the state density function of energies.

This is the reason for calling Z the "partition function": it encodes how the probabilities are partitioned among the different microstates, based on their individual energies. The letter Z stands for the German word Zustandssumme, "sum over states". The usefulness of the partition function stems from the fact that it can be used to relate macroscopic thermodynamic quantities to the microscopic details of a system through the derivatives of its partition function. Finding the partition function is also equivalent to performing a Laplace transform of the density of states function from the energy domain to the β domain, and the inverse Laplace transform of the partition function reclaims the state density function of energies.

## Grand canonical partition function

We can define a grand canonical partition function for a grand canonical ensemble, which describes the statistics of a constant-volume system that can exchange both heat and particles with a reservoir. The reservoir has a constant temperature T, and a chemical potential μ.

We can define a grand canonical partition function for a grand canonical ensemble, which describes the statistics of a constant-volume system that can exchange both heat and particles with a reservoir. The reservoir has a constant temperature T, and a chemical potential μ.

The grand canonical partition function, denoted by $\displaystyle{ \mathcal{Z} }$, is the following sum over microstates

$\displaystyle{ \mathcal{Z}(\mu, V, T) = \sum_{i} \exp\left(\frac{N_i\mu - E_i}{k_B T} \right). }$

(mu，v，t) = sum _ { i } exp left (frac { n _ i mu-e _ i }{ k _ b _ t } right) .数学

The grand canonical partition function, denoted by $\displaystyle{ \mathcal{Z} }$, is the following sum over microstates

Here, each microstate is labelled by $\displaystyle{ i }$, and has total particle number $\displaystyle{ N_i }$ and total energy $\displaystyle{ E_i }$. This partition function is closely related to the grand potential, $\displaystyle{ \Phi_{\rm G} }$, by the relation

$\displaystyle{ \mathcal{Z}(\mu, V, T) = \sum_{i} \exp\left(\frac{N_i\mu - E_i}{k_B T} \right). }$

$\displaystyle{ -k_B T \ln \mathcal{Z} = \Phi_{\rm G} = \langle E \rangle - TS - \mu \langle N\rangle. }$

Here, each microstate is labelled by $\displaystyle{ i }$, and has total particle number $\displaystyle{ N_i }$ and total energy $\displaystyle{ E_i }$. This partition function is closely related to the grand potential, $\displaystyle{ \Phi_{\rm G} }$, by the relation

This can be contrasted to the canonical partition function above, which is related instead to the Helmholtz free energy.

$\displaystyle{ -k_B T \ln \mathcal{Z} = \Phi_{\rm G} = \langle E \rangle - TS - \mu \langle N\rangle. }$

This can be contrasted to the canonical partition function above, which is related instead to the Helmholtz free energy.

It is important to note that the number of microstates in the grand canonical ensemble may be much larger than in the canonical ensemble, since here we consider not only variations in energy but also in particle number. Again, the utility of the grand canonical partition function is that it is related to the probability that the system is in state $\displaystyle{ i }$:

$\displaystyle{ p_i = \frac{1}{\mathcal Z} \exp\left(\frac{N_i\mu - E_i}{k_B T}\right). }$

{ mathcal z } exp left (frac { n _ i mu-e _ i }{ k _ b t } right) . </math >

It is important to note that the number of microstates in the grand canonical ensemble may be much larger than in the canonical ensemble, since here we consider not only variations in energy but also in particle number. Again, the utility of the grand canonical partition function is that it is related to the probability that the system is in state $\displaystyle{ i }$:

$\displaystyle{ p_i = \frac{1}{\mathcal Z} \exp\left(\frac{N_i\mu - E_i}{k_B T}\right). }$

An important application of the grand canonical ensemble is in deriving exactly the statistics of a non-interacting many-body quantum gas (Fermi–Dirac statistics for fermions, Bose–Einstein statistics for bosons), however it is much more generally applicable than that. The grand canonical ensemble may also be used to describe classical systems, or even interacting quantum gases.

An important application of the grand canonical ensemble is in deriving exactly the statistics of a non-interacting many-body quantum gas (Fermi–Dirac statistics for fermions, Bose–Einstein statistics for bosons), however it is much more generally applicable than that. The grand canonical ensemble may also be used to describe classical systems, or even interacting quantum gases.

The grand partition function is sometimes written (equivalently) in terms of alternate variables as

$\displaystyle{ \mathcal{Z}(z, V, T) = \sum_{N_i} z^{N_i} Z(N_i, V, T), }$

< math > mathcal { z }(z，v，t) = sum _ { n _ i } z (n _ i，v，t) ，</math >

The grand partition function is sometimes written (equivalently) in terms of alternate variables as[2]

where $\displaystyle{ z \equiv \exp(\mu/kT) }$ is known as the absolute activity (or fugacity) and $\displaystyle{ Z(N_i, V, T) }$ is the canonical partition function.

$\displaystyle{ \mathcal{Z}(z, V, T) = \sum_{N_i} z^{N_i} Z(N_i, V, T), }$

where $\displaystyle{ z \equiv \exp(\mu/kT) }$ is known as the absolute activity (or fugacity) and $\displaystyle{ Z(N_i, V, T) }$ is the canonical partition function.

## References

1. Klauder, John R.; Skagerstam The classical form of Z is recovered when the trace is expressed in terms of coherent states 当轨迹用相干态表示时，恢复了 z 的经典形式, Bo-Sture (1985). Coherent States: Applications in Physics and Mathematical Physics and when quantum-mechanical uncertainties in the position and momentum of a particle 当粒子位置和动量的量子力学不确定性. World Scientific. pp. 71–73. ISBN 978-9971-966-52-2.
2. Baxter, Rodney J. (1982). Exactly solved models in statistical mechanics. Academic Press Inc.. ISBN 9780120831807.
• Huang, Kerson, "Statistical Mechanics", John Wiley & Sons, New York, 1967.
• A. Isihara, "Statistical Physics", Academic Press, New York, 1971.
• L. D. Landau and E. M. Lifshitz, "Statistical Physics, 3rd Edition Part 1", Butterworth-Heinemann, Oxford, 1996.

Category:Concepts in physics

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