In a first course on statistical mechanics the partition function is normally introduced as the normalisation for the probability of a particle being in a particular energy level. $$p_j=\frac{1}{Z}\exp\left(\frac{-E_j}{k_bT}\right),$$ $$Z=\sum_j \exp\left(\frac{-E_j}{k_bT}\right).$$ Through various manipulations (taking derivatives and so on) we can recover the macroscopic thermodynamic variables of the system. It seems a little fortuitous to me that without specificing more than $Z$ we can recover so much information about our system especially when it is introduced as normalisation.

Is there a better way to view the partition function other than the normalisation of probabilites? It just seems pretty amazing that it has so much information encoded about the system when really all it does is ensure that $\sum_j p_j=1.$


4 Answers 4


The partition function is strongly related to a very useful tool in probability theory called the moment generating function(al) of the probability distribution.

For any probability distribution $p$ of some random variable $X$, the generating function $\mathcal{M}(z)$ is defined as being:

\begin{equation} \mathcal{M}(z) \equiv \left\langle e^{zX}\right\rangle \end{equation}

so that we have for instance:

\begin{equation} \left(\frac{\partial \mathcal{M}}{\partial z}\right)_{z = 0} = \langle X \rangle, \end{equation}

\begin{equation} \left(\frac{\partial^2 \mathcal{M}}{\partial z^2}\right)_{z = 0} = \langle X^2 \rangle, \end{equation} and in general \begin{equation} \mathcal{M}^{(n)}(0) = \langle X^n \rangle \end{equation}

Now, in statistical mechanics the canonical ensembles (with the exception of the microcanonical ensemble) have an exponential form with respect to their corresponding fluctuating thermodynamic random variables (the energy $E$ for the canonical ensemble, the energy $E$ and the number of particles $N$ for the grand canonical ensemble and the energy $E$ and the volume $V$ for the isobaric ensemble, to name a few) so that the probability distribution itself has a form like this

\begin{equation} p_t(X) = f(X)e^{tX} \end{equation}where $t$ is a real number corresponding to one of the intensive thermodynamic variables.

The moment generating function for probabilities like these will look like

\begin{equation} \mathcal{M}(z) =\left \langle e^{zX}\right\rangle = \int \mathrm d\mu(x) \:f(x) e^{tx} e^{zx} \end{equation}

It is quite easy to realize that if we define a partition function as being

\begin{equation} Z(t) \equiv \int \mathrm d\mu(x) \: f(x)e^{tx}, \end{equation} we find that

\begin{equation} \mathcal{M}(z) = Z(t+z) \end{equation}so that

\begin{equation} \mathcal{M}^{(n)}(0) = Z^{(n)}(t) \end{equation}

In general in statistical mechanics, we prefer looking at the log of the partition function (which is also incidentally the logarithm of the moment generating function) as it allows to generate the cumulants of the distribution instead of the moments by applying successive derivatives.

  • 8
    $\begingroup$ One might also mention that the moment generating function is essentially the Laplace transform of the probability distribution, which (if the reader is familiar with Laplace transforms) explains why information isn't lost in calculating it. $\endgroup$
    – N. Virgo
    Apr 5, 2015 at 11:25
  • $\begingroup$ @N.Virgo very interesting comment about information, probably it should be added to the "Meaning" section in Wiki, where there is the "Laplace transform interpretation", en.wikipedia.org/wiki/… $\endgroup$
    – Quillo
    Mar 2 at 10:21

The partition function contains so much information because it is directly related to the free energy, $$F = - k_B T \ln(Z) \, .$$ The physical assumption behind considering $F$ as a thermodynamic potential is that the statistics of the system as described by the canonical ensemble.

In turn, the applicability of the canonical ensemble is a direct consequence of the applicability of the microcanonical ensemble. The microcanonical ensemble states that all micro-states with identical energies will be visited by the dynamics of the system equally. This is called the ergodicity hypothesis. It works so well because most realistic systems are chaotic.

To summarise, the reasonning goes as follows:

Systems are chaotic $\rightarrow$ Microcanonical ensemble works, the entropy is a thermodynamic potential $\rightarrow$ Legendre transform the entropy implies that the free energy is a thermodynamic potential $\rightarrow$ The free energy is given by $F=-k_b T \ln(Z)$ $\rightarrow$ $Z$ contains all the thermodynamic information that one can wish for.

At the level of the thermodynamic potentials, entropy and free energy are related through a Legendre transform, $$S(E) \rightarrow F(T) = S(E(T))-T E(T)\, .$$ At the level of statistical physics, this is mirrored in the relation $$Z = \sum_{E} \Omega(E) \text{e}^{-E/k_BT} \, .$$ $\Omega(E)$ is the microcanonical "partition function". It is the number of micro-states with energy $E$ and is related to the entropy through $$ S(E) = k_B\ln(\Omega(E)) \, .$$

Note that in your expression for $Z$, you sum over all the micro-states of the system. Here I sum over the different energies that the system may have and use $\Omega(E)$ as a weight factor.


I think one way to understand why this works is that the spectrum of energy levels $E_i$ has undergone a sort of transform (analogous to Laplace transform) which results in the partition function $Z(T)$. In principle if you know the function $Z(T)$ you can reverse the process, and reconstruct the original spectrum of energy levels.

As such, all information about the $E_i$ spectrum has been encoded into $Z(T)$.


You can think of partition function as a statistical description of an ensemble. Suppose you have a closed system S where the i.th microstate has energy $E_i$. Your partition function, $p_i$ of the ensemble will be proportional to total number of microstates of the heat bath, $\Omega(E-E_i)$. For heat bath $E \gg E_i$ Taylor expand $\Omega$ around $E_i$, $$ S=k\log(p_i)\sim k\log\Omega(E-E_i)= k\log\Omega(E)-\frac{\partial( k\log\Omega(E))}{\partial E}E_i $$ $$ =k\log\Omega(E)-\frac{\partial S}{\partial E}E_i=k\log\Omega(E)-\frac{E_i}{kT} $$ $$ p_i\sim\exp\left(-\frac{E_i}{kT}+\log\Omega(E)\right)=\Omega(E)\exp\left(-\frac{E_i}{kT}\right) $$ so the probability $p_i$ of the system being $\rm i^{th}$ state proportional to the partition function. If the microstates of your ensemble are not equally probable you need to use Gibbs entropy $S=-k\sum p_ilog(p_i)$, but if all of them are likely to occur this reduces to Boltzmann entropy. You can see it easily with a probability $$ p_i=\frac{1}{\Omega(E)} $$ for each microstates ($\sum p_i=1$).


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