Gibbs measure

In physics and mathematics, the Gibbs measure, named after Josiah Willard Gibbs, is a probability measure frequently seen in many problems of probability theory and statistical mechanics. It is a generalization of the canonical ensemble to infinite systems. The canonical ensemble gives the probability of the system X being in state x (equivalently, of the random variable X having value x) as

P(X=x)={\frac {1}{Z(\beta )}}\exp(-\beta E(x)).

Here, $E$ is a function from the space of states to the real numbers; in physics applications, $E (x)$ is interpreted as the energy of the configuration x. The parameter $β$ is a free parameter; in physics, it is the inverse temperature. The normalizing constant $Z (β)$ is the partition function. However, in infinite systems, the total energy is no longer a finite number and cannot be used in the traditional construction of the probability distribution of a canonical ensemble. Traditional approaches in statistical physics studied the limit of intensive properties as the size of a finite system approaches infinity (the thermodynamic limit). When the energy function can be written as a sum of terms that each involve only variables from a finite subsystem, the notion of a Gibbs measure provides an alternative approach. Gibbs measures were proposed by probability theorists such as Dobrushin, Lanford, and Ruelle and provided a framework to directly study infinite systems, instead of taking the limit of finite systems.

A measure is a Gibbs measure if the conditional probabilities it induces on each finite subsystem satisfy a consistency condition: if all degrees of freedom outside the finite subsystem are frozen, the canonical ensemble for the subsystem subject to these boundary conditions matches the probabilities in the Gibbs measure conditional on the frozen degrees of freedom.

The Hammersley–Clifford theorem implies that any probability measure that satisfies a Markov property is a Gibbs measure for an appropriate choice of (locally defined) energy function. Therefore, the Gibbs measure applies to widespread problems outside of physics, such as Hopfield networks, Markov networks, Markov logic networks, and boundedly rational potential games in game theory and economics. A Gibbs measure in a system with local (finite-range) interactions maximizes the entropy density for a given expected energy density; or, equivalently, it minimizes the free energy density.

The Gibbs measure of an infinite system is not necessarily unique, in contrast to the canonical ensemble of a finite system, which is unique. The existence of more than one Gibbs measure is associated with statistical phenomena such as symmetry breaking and phase coexistence.

Statistical physics

The set of Gibbs measures on a system is always convex,^[1] so there is either a unique Gibbs measure (in which case the system is said to be "ergodic"), or there are infinitely many (and the system is called "nonergodic"). In the nonergodic case, the Gibbs measures can be expressed as the set of convex combinations of a much smaller number of special Gibbs measures known as "pure states" (not to be confused with the related but distinct notion of pure states in quantum mechanics). In physical applications, the Hamiltonian (the energy function) usually has some sense of locality, and the pure states have the cluster decomposition property that "far-separated subsystems" are independent. In practice, physically realistic systems are found in one of these pure states.

If the Hamiltonian possesses a symmetry, then a unique (i.e. ergodic) Gibbs measure will necessarily be invariant under the symmetry. But in the case of multiple (i.e. nonergodic) Gibbs measures, the pure states are typically not invariant under the Hamiltonian's symmetry. For example, in the infinite ferromagnetic Ising model below the critical temperature, there are two pure states, the "mostly-up" and "mostly-down" states, which are interchanged under the model's $\mathbb {Z} _{2}$ symmetry.

Markov property

An example of the Markov property can be seen in the Gibbs measure of the Ising model. The probability for a given spin $σ k$ to be in state s could, in principle, depend on the states of all other spins in the system. Thus, we may write the probability as

P(\sigma _{k}=s\mid \sigma _{j},\,j\neq k)

.

However, in an Ising model with only finite-range interactions (for example, nearest-neighbor interactions), we actually have

P(\sigma _{k}=s\mid \sigma _{j},\,j\neq k)=P(\sigma _{k}=s\mid \sigma _{j},\,j\in N_{k})

,

where $N k$ is a neighborhood of the site $k$ . That is, the probability at site $k$ depends only on the spins in a finite neighborhood. This last equation is in the form of a local Markov property. Measures with this property are sometimes called Markov random fields. More strongly, the converse is also true: any positive probability distribution (nonzero density everywhere) having the Markov property can be represented as a Gibbs measure for an appropriate energy function.^[2] This is the Hammersley–Clifford theorem.

Formal definition on lattices

What follows is a formal definition for the special case of a random field on a lattice. The idea of a Gibbs measure is, however, much more general than this.

The definition of a Gibbs random field on a lattice requires some terminology:

The lattice: A countable set $\mathbb {L}$ .
The single-spin space: A probability space $(S,{\mathcal {S}},\lambda )$ .
The configuration space: $(\Omega ,{\mathcal {F}})$ , where $\Omega =S^{\mathbb {L} }$ and ${\mathcal {F}}={\mathcal {S}}^{\mathbb {L} }$ .
Given a configuration $ω \in Ω$ and a subset $\Lambda \subset \mathbb {L}$ , the restriction of $ω$ to $Λ$ is $\omega _{\Lambda }=(\omega (t))_{t\in \Lambda }$ . If $\Lambda _{1}\cap \Lambda _{2}=\emptyset$ and $\Lambda _{1}\cup \Lambda _{2}=\mathbb {L}$ , then the configuration $\omega _{\Lambda _{1}}\omega _{\Lambda _{2}}$ is the configuration whose restrictions to $Λ 1$ and $Λ 2$ are $\omega _{\Lambda _{1}}$ and $\omega _{\Lambda _{2}}$ , respectively.
The set ${\mathcal {L}}$ of all finite subsets of $\mathbb {L}$ .
For each subset $\Lambda \subset \mathbb {L}$ , ${\mathcal {F}}_{\Lambda }$ is the $σ$ -algebra generated by the family of functions $(\sigma (t))_{t\in \Lambda }$ , where $\sigma (t)(\omega )=\omega (t)$ . The union of these $σ$ -algebras as $\Lambda$ varies over ${\mathcal {L}}$ is the algebra of cylinder sets on the lattice.
The potential: A family $\Phi =(\Phi _{A})_{A\in {\mathcal {L}}}$ of functions Φ_A : Ω → R such that
1. For each $A\in {\mathcal {L}},\Phi _{A}$ is ${\mathcal {F}}_{A}$ -measurable, meaning it depends only on the restriction $\omega _{A}$ (and does so measurably).
2. For all $\Lambda \in {\mathcal {L}}$ and $ω \in Ω$ , the following series exists:^{[when defined as?]}

H_{\Lambda }^{\Phi }(\omega )=\sum _{A\in {\mathcal {L}},A\cap \Lambda \neq \emptyset }\Phi _{A}(\omega ).

We interpret $Φ A$ as the contribution to the total energy (the Hamiltonian) associated to the interaction among all the points of finite set A. Then $H_{\Lambda }^{\Phi }(\omega )$ as the contribution to the total energy of all the finite sets A that meet $\Lambda$ . Note that the total energy is typically infinite, but when we "localize" to each $\Lambda$ it may be finite, we hope.

The Hamiltonian in $\Lambda \in {\mathcal {L}}$ with boundary conditions ${\bar {\omega }}$ , for the potential $Φ$ , is defined by

H_{\Lambda }^{\Phi }(\omega \mid {\bar {\omega }})=H_{\Lambda }^{\Phi }\left(\omega _{\Lambda }{\bar {\omega }}_{\Lambda ^{c}}\right)

where

\omega _{\Lambda }{\bar {\omega }}_{\Lambda ^{c}}

denotes the configuration taking the values of

\omega

in

\Lambda

, and those of

{\bar {\omega }}

in

\Lambda ^{c}:=\mathbb {L} \setminus \Lambda

.

The partition function in $\Lambda \in {\mathcal {L}}$ with boundary conditions ${\bar {\omega }}$ and inverse temperature $β > 0$ (for the potential $Φ$ and $λ$ ) is defined by

Z_{\Lambda }^{\Phi }({\bar {\omega }})=\int \lambda ^{\Lambda }(\mathrm {d} \omega )\exp(-\beta H_{\Lambda }^{\Phi }(\omega \mid {\bar {\omega }})),

where

\lambda ^{\Lambda }(\mathrm {d} \omega )=\prod _{t\in \Lambda }\lambda (\mathrm {d} \omega (t)),

is the product measure

A potential

Φ

is

λ

-admissible if

Z_{\Lambda }^{\Phi }({\bar {\omega }})

is finite for all

\Lambda \in {\mathcal {L}},{\bar {\omega }}\in \Omega

and

β > 0

.

A probability measure

μ

on

(\Omega ,{\mathcal {F}})

is a Gibbs measure for a

λ

-admissible potential

Φ

if it satisfies the Dobrushin–Lanford–Ruelle (DLR) equation

\int \mu (\mathrm {d} {\bar {\omega }})Z_{\Lambda }^{\Phi }({\bar {\omega }})^{-1}\int \lambda ^{\Lambda }(\mathrm {d} \omega )\exp(-\beta H_{\Lambda }^{\Phi }(\omega \mid {\bar {\omega }}))\,1_{A}(\omega _{\Lambda }{\bar {\omega }}_{\Lambda ^{c}})=\mu (A),

for all

A\in {\mathcal {F}}

and

\Lambda \in {\mathcal {L}}

.

An example

To help understand the above definitions, here are the corresponding quantities in the important example of the Ising model with nearest-neighbor interactions (coupling constant $J$ ) and a magnetic field ( $h$ ), on $Z d$ :

The lattice is simply $\mathbb {L} =\mathbf {Z} ^{d}$ .
The single-spin space is $S = {-1, 1}.$
The potential is given by

\Phi _{A}(\omega )={\begin{cases}-J\,\omega (t_{1})\omega (t_{2})&{\text{if }}A=\{t_{1},t_{2}\}{\text{ with }}\|t_{2}-t_{1}\|_{1}=1\\-h\,\omega (t)&{\text{if }}A=\{t\}\\0&{\text{otherwise}}\end{cases}}

References

^ "Gibbs measures" (PDF).
^ Ross Kindermann and J. Laurie Snell, Markov Random Fields and Their Applications (1980) American Mathematical Society, ISBN 0-8218-5001-6

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