In colloidal solutions, a widely-used relation connects the scale-dependent collective diffusion constant and the structure factor:

\begin{equation}D_c(q) =\frac{D_0}{S(q)}

\label{eq:dGn}

\end{equation} and is generally known as

*de Gennes narrowing*since its use by de Gennes in the context of quasi-elastic neutron scattering from liquids [1].

Intuitively, equation \eqref{eq:dGn} makes sense: if \(S(q)\) is high for a certain value of \(q\) then fluctuations with that particular \(q\) are frequent, meaning that their energetic cost is low and that they will decay slowly. However, I have not yet found in the literature a simple yet rigorous derivation. This is what I will attempt below.

Consider a system characterized by a conserved scalar parameter \( \phi(\mathbf{r})\) (for instance, the local particle concentration in a suspension). The free energy only depends on this field: \(\mathcal{F}[\phi(\mathbf{r})]\) or, equvalently, on its Fourier components: \(\mathcal{F}[\phi(\mathbf{q})]\).

For an isotropic system in the absence of applied fields, all fluctuations \( \phi(\mathbf{q})\) with \( \left |\mathbf{q} \right | > 0\) will eventually decay to zero. To fix the ideas, we will consider an overdamped relaxation (model B in the Hohenberg-Halperin classification [2], but of course far from criticality).

Let us write Fick's laws, with \( \mathbf{j} \) and \( \mu\) the current and chemical potential associated to \( \phi\) (this is similar to the presentation in [2], Eqs. (2.2)-(2.9)):

\[ \frac{\partial \phi(\mathbf{r},t)}{\partial t} = - \nabla \mathbf{j} \, ; \quad \mathbf{j} = - \lambda \nabla \mu \, ; \quad \mu = \frac{\delta \mathcal{F}}{\delta \phi(\mathbf{r},t)} \, \Rightarrow \, \frac{\partial \phi(\mathbf{r},t)}{\partial t} = \lambda \nabla ^2 \frac{\delta \mathcal{F}}{\delta \phi(\mathbf{r},t)}\] where \( \delta\) denotes the functional derivative. Introducing the Fourier components yields: \begin{equation}

\label{eq:relax}

\frac{\partial \phi(\mathbf{r},t)}{\partial t}= \lambda \nabla ^2 \frac{\delta \mathcal{F}}{\delta \phi(\mathbf{r},t)} \Rightarrow \frac{\partial \phi(\mathbf{q},t)}{\partial t} = - \lambda q^2 \frac{\text{d} \mathcal{F}}{\text{d}\phi(\mathbf{q},t)}

\end{equation} If the different Fourier modes are uncoupled, we can write the equipartition relation:

\begin{equation}

\label{eq:equi}

\mathcal{F} = \sum_{\mathbf{q}} \frac{A(\mathbf{q})}{2} \phi(\mathbf{q}) ^2 \Rightarrow \frac{\text{d} \mathcal{F}}{\text{d}\phi(\mathbf{q},t) } = A(\mathbf{q}) \phi(\mathbf{q})

\end{equation} From \eqref{eq:relax} and \eqref{eq:equi}, the evolution of mode \(\mathbf{q}\) is given by: \begin{equation}

\label{eq:evol}

\frac{\partial \phi(\mathbf{q},t)}{\partial t}=- \lambda q^2 A(\mathbf{q}) \phi(\mathbf{q,t}) \Rightarrow \frac{\phi(q,t)}{\phi(\mathbf{q},0)} = \exp \left \lbrace - D_c(q) q^2 t \right \rbrace

\end{equation} where we invoked the isotropy of the system. The collective diffusion coefficient is given by: \begin{equation}

\label{eq:Dc}

D_c(q) = \lambda A(q)

\end{equation} On the other hand,equipartition also implies: \begin{equation}

S(\mathbf{q}) = \left \langle \phi(\mathbf{q}) \phi(\mathbf{-q}) \right \rangle = \frac{k_B T}{A(\mathbf{q})}

\label{eq:Sq}

\end{equation} with \( \left \langle \cdot \right \rangle\) the ensemble average. From \eqref{eq:Dc} and \eqref{eq:Sq} we finally obtain:

\begin{equation}

\label{eq:final}

D_c(q) = \frac{\lambda k_B T}{S(q)}

\end{equation}

For simplicity's sake I glossed over some technical details, such as the proper use of \( \phi(\mathbf{q})\) and \( \phi(\mathbf{-q})\) and the rigorous form of the time evolution in Eq. \eqref{eq:evol}.

[1] P. G. de Gennes, Liquid dynamics and inelastic scattering of neutrons,

*Physica A*

**25**, 825-839 (1959).

[2] P. C. Hohenberg and B. Halperin, Theory of dynamic critical phenomena,

*Rev. Mod. Phys.*

**49**, 435-479 (1977).

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