## 1.2 The General Heat Equation

We can further generalize our previous problem and replace $\Delta$ by any elliptic self-adjoint operator. We will soon specialize to the case of the Laplace–Beltrami operator, but this section is completely general.

Our original motivation was to understand the index of operators, so let us start from there. Suppose we are given a compact Riemannian manifold $M$ and $E, F$ Hermitian vector bundles on $M$. We are also given an elliptic differential operator $D\colon \Gamma (E) \to \Gamma (F)$ over $M$ with formal adjoint $D^*\colon \Gamma (F) \to \Gamma (E)$ (in the case of the Laplace–Beltrami operator, we have $D = D^* = \mathrm{d}+ \mathrm{d}^*$ and $E = F = \Omega ^*$).

Similar to the case of the Laplace–Beltrami operator, we define

$\begin{aligned} \Delta _ E & = D^* D \colon \Gamma (E) \to \Gamma (E)\\ \Delta _ F & = D D^*\colon \Gamma (F) \to \Gamma (F). \end{aligned}$Then $\ker \Delta _ E = \ker D$ and $\ker \Delta _ F = \ker D^*$. So we have

$\begin{aligned} \operatorname{index}D & = \dim \ker D - \dim \operatorname{coker}D \\ & = \dim \ker D - \dim \ker D^*\\ & = \dim \ker \Delta _ E - \dim \ker \Delta _ F. \end{aligned}$This is the form of the index that will be of interest to us.

By analogy with the classical heat equation, we consider the equation

$\left(\frac{\partial }{\partial t} + \Delta _ E\right) f = 0$on $E \times (0, \infty ) \to M \times (0, \infty )$, with $t \in (0, \infty )$.

Hodge theory gives us an easy way to solve this, at least formally. We can decompose

$L^2(E) = \bigoplus _\lambda \Gamma _\lambda (E),$where $\Gamma _\lambda (E)$ is the $\lambda$-eigenspace of $\Delta _ E$. The spectral theorem tells us the eigenvalues are discrete and tend to infinity. Let $\{ \psi _\lambda \}$ be an orthonormal eigenbasis. Then we can write a general solution as

$f(x, t) = \sum _\lambda c_\lambda e^{-\lambda t} \psi _\lambda (x)$for some constants $c_\lambda$.

If we want to solve this with initial condition $f_0$, i.e. we require $f(-, t) \to f_0$ as $t \to 0$ in $L^2$, then we must pick
^{1}

Thus, we can write the heat kernel as

$H_ t(x, y; \Delta _ E) = \sum _\lambda e^{\lambda t} \psi _\lambda (x) \psi _\lambda (y)^ T.$Then we have

$f(x, t) = \int _ M H_ t(x, y; \Delta _ E) f_0(y)\; \mathrm{d}y.$We remark that for each fixed $t$, the heat kernel $H_ t(x, y)$ is a section of the exterior product $E \boxtimes E^* \to M \times M$.

To ensure the sum converges, we need to make sure the eigenvalues grow sufficiently quickly. This is effectively Weyl's law, but we for our purposes, we can use a neat trick to obtain a weaker bound easily.

If $\Delta$ is any self-adjoint elliptic differential operator, then there is a constant $C$ and an exponent $\varepsilon$ such that for large $\Lambda$, the number of eigenvalues of magnitude $\leq \Lambda$ is at most $C \Lambda ^\varepsilon$.

Elliptic regularity lets us bound the higher Sobolev norms of $H_ t$ as well, and so we know $H_ t$ is in fact smooth by Sobolev embedding.

It is fruitful to consider the “time evolution” operator $e^{-t \Delta _ E}$ that sends $f_0$ to $f(-, t)$ defined above. This acts on the $\lambda$ eigenspace by multiplication by $e^{-\lambda t}$. Thus, the trace is given by

$h_ t(\Delta _ E) \equiv \operatorname{tr}e^{-t \Delta _ E} = \sum _\lambda e^{-\lambda t} \dim \Gamma _\lambda (E).$The key observation is that $D$ gives an isomorphism between the $\lambda$ eigenspace of $\Delta _ E$ and the $\lambda$ eigenspace of $\Delta _ F$ as long as $\lambda > 0$, and the $0$ eigenspaces are exactly the kernels of $\Delta _ E$ and $\Delta _ F$. So we have an expression

$\operatorname{index}\Delta _ E = h_ t(\Delta _ E) - h_ t(\Delta _ F)$for any $t > 0$.

This expression is a very global one, because $h_ t(\Delta _ E)$ depends on the eigenfunctions of $\Delta _ E$. However, the fact that $e^{-\lambda \Delta _ E}$ is given by convolution with $H_ t(x, y; \Delta _ E)$ gives us an alternative expression for the trace, namely

$h_ t(\Delta _ E) = \int _ M H_ t(x, x; \Delta _ E)\; \mathrm{d}x.$This is still non-local, but we will later find that the asymptotic behaviour of $H_ t(x, x; \Delta _ E)$ as $t \to 0$ is governed by local invariants. Since the index is independent of $t$, we can take the limit $t \to 0$ and get a local expression for the index.

Take the flat torus $T^ d = \mathbb {R}^ d / \mathbb {Z}^ d$, and pick $D = \mathrm{d}\colon \Omega ^0(M) \to \Omega ^1(M)$, so that $\Delta$ is the classical Laplacian

$\Delta = -\sum \frac{\partial ^2}{\partial x_ i^2}.$The eigenvectors are given by $e^{2\pi ix\cdot \xi }$ for $\xi \in \mathbb {Z}^ d$ with eigenvalue $4\pi ^2 |\xi |^2$. So the heat kernel is

$H_ t(x, y) = \sum _{\xi \in \mathbb {Z}^ d} e^{-4\pi t |\xi |^2} e^{2\pi i(x - y)\cdot \xi } = \prod _{i = 1}^ d \sum _{k = -\infty }^\infty e^{-4 \pi t k^2 + 2 \pi i (x_ i - y_ i) k}.$Number theorists may wish to express this in terms of the Jacobi theta function:

$H_ t(x, y) = \prod _{i = 1}^ d \vartheta (x_ i - y_ i; 4it).$We can explicitly evaluate the trace to be

$h_ t = \int _{T^ d} H_ t(x, x) \; \mathrm{d}x = \left(\sum _{k = -\infty }^\infty e^{-4\pi t k^2}\right)^ d$In the limit $t \to 0$, we can replace the sum with the integral to get

$h_ t \sim \left(\int _{-\infty }^\infty e^{-4\pi t k^2}\; \mathrm{d}k\right)^ d = (4t)^{-d/2}.$