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*Landau theory*

is an effort to describe all phase transitions from various fields within
physics using a uniform approach. This should be
independent of which state variable drives the system

across a phase boundary, and it should also apply
irrespective of what feature of the system is being (dis)ordered

(atoms, chemical bonds, magnetic moments...) in the process. Naturally, this requires a
high level of abstraction from the underlying physics. Landau theory was devised specifically for
second-order phase transitions,

but it can be applied to first-order transitions without introducing a
significant amount of error.

The fundamental idea of Landau theory is to define an
*order parameter, Q* (or sometimes ζ),

*i.e.* a
measurable property that traces a system's approach to a phase transition.

Many different physical properties can be used as an order parameter for different kinds of transition,
and usually there are different properties which could equally well be used for a given transition. The point
is that it is something that varies sharply at the transition point and can be measured easily. Examples
include:

- density As we have seen, the increase in symmetry in the high-temperature phase during crystallographic transitions leads to a reduction in density. Therefore density can be used as an order parameter for such transitions.
- site occupancies Site occupancies can be measured indirectly, for example by phonon spectroscopy. If a site becomes vacant or is only occupied part of the time on the high-temperature side of a displacive transition, the occupancy fraction can be used as an order parameter.
- Bragg peak intensities Diffraction peaks disappear as a consequence of systematic absences
- Bragg peak positions If inter-atomic distances change during a phase transition, Bragg peaks will move as a result.
- magnetisation, polarisation In transitions between ferromagnetic and paramagnetic states (or their electrical analogues), the magnetisation (polarisation) will vanish abruptly because the individual magnetic moment (dipole moment) vectors cancel out in the disordered phase, making a good order parameter.
- resistivity Resistivity is a useful order parameter in transitions involving superconductors since it vanishes below the transition point.
- ...

in the case of centred unit cells. Therefore, Bragg peaks will vanish during a displacive phase transition if the high-temperature phase has a centred lattice (as in the example discussed).

In order for all these different observable properties to be used as order parameters, they
need to be
*scaled* to be within $[0\cdots 1]$,

where $Q=0$ corresponds to the ordered phase. Below the transition, in the disordered phase
the order parameter rises to its low-temperature limit of 1. For example, in the case of
the displacive transition shown, the distance of the atom from the centre position along the
diagonal (as measured by Bragg angle) is 0 in the high-temperature phase and gradually increases
upon cooling below $T_c$ as the atom settles in its asymmetric potential well.

The order parameter is normalised in such a way that $Q=0$ above the transition and $Q=1$ in the limit of $T\to\mathrm{0\,K}$. The free enthalpy of the thermodynamically stable phase has a minimum at the value of the order parameter for the given temperature (or whichever state variable is being changed). As a result, we have

- $T\gt T_c$: one minimum at $Q=0$
- $T\lt T_c$: two minima at $|Q|\gt 0$

For a symmetric problem such as the displacement of an atom along the cell diagonal,
*Taylor expansion* of the free enthalpy

produces
$$G(Q)=G_0+\frac{1}{2}aQ^2+\frac{1}{4}bQ^4+\cdots$$
In a second-order phase transition, the coefficient of the second-order expansion term
$a$ varies smoothly with temperature and hinges on $T_c$:

$$a(T)=a_0(T-T_c)\qquad,$$
*i.e.* the strength of the term depends on how far away from the transition temperature $T_c$
the system is. By inserting this into the expanded $G(Q)$ expression, we have:
$$G(Q)=G_0+\frac{1}{2}a_0(T-T_c)Q^2+\frac{1}{4}bQ^4+\cdots$$
We find the minima and maxima of $G(Q)$ by finding the points where its derivative is zero:
$$\frac{\partial G}{\partial Q}=a_0(T-T_c)Q+bQ^3\overset{!}{=}0$$
This produces the
solutions:

$$Q=0\textrm{ - minimum for }T\gt T_c\textrm{, maximum for }T\lt T_c\textrm{, and}$$
$$Q=\pm\sqrt{\frac{a_0}{b}(T_c-T)}\textrm{ - unphysical (since imaginary) for }T\gt T_c\textrm{, minima for }T\lt T_c\textrm{.}$$
Therefore, we can see that the two free energy minima gradually move towards $Q=0$ as the system heats
up towards $T_c$. From $T_c$ onwards, the free energy minimum remains fixed at $Q=0$, indicative of
the high-temperature, high-symmetry phase.

Clearly this approach produces the required temperature dependence of the order parameter: At the lowest temperatures, $Q$ approaches one, falling gradually towards zero at $T_c$. The rate of change increases as the phase transition is approached. Above the transition point, the order parameter remains fixed at zero.

In a first-order phase transition, the order parameter drops to zero instantly at the transition
point after gradually decreasing somewhat from the low-temperature limit of one. The difficulty
in determining the order of a phase transition experimentally is mirrored here: with finite
precision of the temperature measurement, it is impossible to tell whether the angle between
the $G(Q)$ function and the temperature axis is 90^{o} (1st order) or marginally larger
(2nd order).

In the following section, we'll explore the predictions of Landau theory for the enthalpy,
entropy and heat capacity changes occurring at a second-order phase transition. The free
enthalpy, which constitutes the balance of the two phases present at the transition, is given by
$$\Delta G=\Delta H-T\Delta S\qquad,$$
where the letter $\Delta$ refers to the change of the state functions as a consequence of the
transition. On the left-hand side, the change of the free enthalpy is equal to the terms that
depend on the order parameter, $Q$, in the series
expansion (as derived in the previous box):
$$\Delta G=G(Q)-G_0=\frac{1}{2}a_0(T-T_c)Q^2+\frac{1}{4}bQ^4+\cdots$$
because $Q=0$ above the transition. Considering that $T$ is the actual temperature while
$T_c$ is a constant, we can split this into a temperature-dependent and a temperature-independent
part:
$$\bbox[lightblue]{\frac{1}{2}a_0TQ^2}\bbox[lightpink]{-\frac{1}{2}a_0T_cQ^2+\frac{1}{4}bQ^4}=\bbox[lightpink]{\Delta H}\bbox[lightblue]{-T\Delta S}\qquad.$$
Taking the temperature-independent parts of both sides of the equation, we get the
*transition enthalpy*:
$$\bbox[lightpink]{\Delta H}=-\frac{1}{2}a_0T_cQ^2+\frac{1}{4}bQ^4\qquad,$$
which produces the familiar double-well function of the order parameter. Meanwhile, the
temperature-dependent terms produce the
*transition entropy*:
$$\bbox[lightblue]{\Delta S}=-\frac{1}{2}a_0Q^2\qquad,$$
*i.e.* a quadratic dependence on the order parameter.

The heat capacity can be calculated from the entropy by evaluating
$$c_p=T\frac{\partial S}{\partial T}\qquad.$$
By using the transition entropy, $\Delta S$, in this formula we can work out the additional
contribution to the heat capacity that results from the phase transition. This is in addition
to the heat capacity of the material itself. Therefore, the
*transition-related component of the heat capacity*

is obtained by evaluating the slope of the entropy at the transition:
$$c_p^{\mathrm{phtr}}=T\frac{\partial(\Delta S)}{\partial T}=-T\frac{1}{2}a_0\frac{\partial Q^2}{\partial T}\qquad.$$
Here we can use the roots of $Q(T)$ we've found above by differentiating the free enthalpy. Below $T_c$, we have found
$$Q(T)=\pm\sqrt{\frac{a_0}{b}(T_c-T)}\qquad\textrm{, so}$$
$$c_p^{\mathrm{phtr}}=-\frac{1}{2}a_0T\frac{\partial}{\partial T}\left(\frac{a_0}{b}(T_c-T)\right)=\frac{a_0^2T}{2b}\qquad.$$
Since $Q(T)=0$ if $T\gt T_c$, the transition-related contribution to $c_p$ above the transition point is zero, *i.e.*
$$\Delta c_p=c_p^{\mathrm{phtr}}$$
determines the size of the step in the heat capacity at the second-order phase transition.

When considering the temperature dependence of the order parameter, $Q(T)$, it is clear
that the function is single-valued only for second-order transitions. For first-order
transitions, the order parameter drops vertically at the transition temperature. Therefore,
the free enthalpy must have at least one additional minimum within the range $[0\dots 1]$ of the
order parameter. This cannot be achieved if the Taylor expansion of $G(Q)$ is truncated after
the quartic ($Q^4$) term. We therefore include the $Q^6$ term as well:
$$G(Q)=\frac{1}{2}a_0(T-T_c)Q^2-\frac{1}{4}bQ^4+\frac{1}{6}cQ^6\qquad .$$
The signs of the expanasion terms alternate, producing the required pattern.

**Note:** Different sources define the coefficients slightly differently,
so the following formulae may look a little different depending on how $a,b,c$ are
introduced.

To find the values of the order parameter at which the free enthalpy is minimal, we need to find the zeroes of the derivative of $G(Q)$ with respect of $Q$: $$\frac{\partial G}{\partial Q}=a_0(T-T_c)Q-bQ^3+cQ^5\stackrel{!}{=}0\qquad .$$

The
solutions

are:
$$Q=0\qquad\textrm{or}$$
$$a_0(T-T_c)-bQ^2+cQ^4=0\qquad .$$
The latter can be solved as a quadratic equation in terms of $Q^2$ as the variable:
$$(Q^2)^2-\frac{b}{c}Q^2+\frac{a_0}{c}(T-T_c)=0\qquad,$$
leading to the solutions
$$Q^2=\frac{b}{2c}\pm\sqrt{\frac{b^2}{4c^2}-\frac{a_0}{c}(T-T_c)}\quad.$$
This can be simplified somewhat by including the $2c$ in the root:
$$Q^2=\frac{1}{2c}\left(b\pm\sqrt{b^2-4a_0c(T-T_c)}\right)\qquad.$$

Since the free energy is a real function, the
inner root must be real, so

$$b^2\ge 4a_0c(T-T_c)\qquad.$$
Solving this for the temperature yields:
$$T\le T_1=T_c+\frac{b^2}{4a_0c}\qquad,$$
where the
*spinodal temperature*, $T_1$,

is the upper limit of the temperature range in which the low-temperature phase can
co-exist as a metastable form alongside the thermodynamically stable high-temperature
phase. In terms of $G(Q)$, this is the point at which a second minimum at $Q\gt 0$
forms. This is a local minimum, *i.e.* the free enthalpy of the high-temperature
phase ($Q=0$) is lower still. At the
*transition temperature*, $T_c$,

the free enthalpy is $G=0$ for both minima, *i.e.* both phases are in thermodynamic
equilibrium. Below the transition temperature, the low-temperature phase becomes stable
while the high-temperature phase can co-exist metastably - its local minimum at $Q=0$
has a larger value than that of the stable phase. At the
*binodal temperature*, $T_0$,

the sign the local minimum of the high-temperature phase flips over and becomes a local
maximum. Below $T_0$, the high-temperature phase cannot exist even as a metastable phase.

Unless terms beyond $Q^6$ are included in the analysis, the two metastable regions are
symmetrical - $T_0$ is as far below $T_c$ as $T_1$ is above it. The metastable regimes
come about because of structural
*fluctuations*

which reach their maximum extent at $T_c$.

The schematic diagram shows the variation of the order parameter with temperature near a first-order phase transition, including the two coexistence regions and the gradual approach to zero of the order parameter of the metastable low-temperature phase as the sample is heated towards the spinodal temperature.

Having established a theoretical framework that applies to all types of phase transitions,
we will next look at experimental approaches to
tracing phase transitions

as they happen.