Our study of random matrices, to date, has focused on somewhat general ensembles, such as iid random matrices or Wigner random matrices, in which the distribution of the individual entries of the matrices was essentially arbitrary (as long as certain moments, such as the mean and variance, were normalised). In these notes, we now focus on two much more special, and much more symmetric, ensembles:

• The Gaussian Unitary Ensemble (GUE), which is an ensemble of random ${n \times n}$ Hermitian matrices ${M_n}$ in which the upper-triangular entries are iid with distribution ${N(0,1)_{\bf C}}$, and the diagonal entries are iid with distribution ${N(0,1)_{\bf R}}$, and independent of the upper-triangular ones; and
• The Gaussian random matrix ensemble, which is an ensemble of random ${n \times n}$ (non-Hermitian) matrices ${M_n}$ whose entries are iid with distribution ${N(0,1)_{\bf C}}$.

The symmetric nature of these ensembles will allow us to compute the spectral distribution by exact algebraic means, revealing a surprising connection with orthogonal polynomials and with determinantal processes. This will, for instance, recover the semi-circular law for GUE, but will also reveal fine spacing information, such as the distribution of the gap between adjacent eigenvalues, which is largely out of reach of tools such as the Stieltjes transform method and the moment method (although the moment method, with some effort, is able to control the extreme edges of the spectrum).

Similarly, we will see for the first time the circular law for eigenvalues of non-Hermitian matrices.

There are a number of other highly symmetric ensembles which can also be treated by the same methods, most notably the Gaussian Orthogonal Ensemble (GOE) and the Gaussian Symplectic Ensemble (GSE). However, for simplicity we shall focus just on the above two ensembles. For a systematic treatment of these ensembles, see the text by Deift.

— 1. The spectrum of GUE —

We have already shown using Dyson Brownian motion in Notes 3b that we have the Ginibre formula

$\displaystyle \rho_n(\lambda) = \frac{1}{(2\pi)^{n/2} 1! \ldots (n-1)!} e^{-|\lambda|^2/2} |\Delta_n(\lambda)|^2 \ \ \ \ \ (1)$

for the density function of the eigenvalues ${(\lambda_1,\ldots,\lambda_n) \in {\bf R}^n_\geq}$ of a GUE matrix ${M_n}$, where

$\displaystyle \Delta_n(\lambda) = \prod_{1 \leq i < j \leq n} (\lambda_i - \lambda_j)$

is the Vandermonde determinant. We now give an alternate proof of this result (omitting the exact value of the normalising constant ${\frac{1}{(2\pi)^{n/2} 1! \ldots (n-1)!}}$) that exploits unitary invariance and the change of variables formula (the latter of which we shall do from first principles). The one thing to be careful about is that one has to somehow quotient out by the invariances of the problem before being able to apply the change of variables formula.

One approach here would be to artificially “fix a gauge” and work on some slice of the parameter space which is “transverse” to all the symmetries. With such an approach, one can use the classical change of variables formula. While this can certainly be done, we shall adopt a more “gauge-invariant” approach and carry the various invariances with us throughout the computation. (For a comparison of the two approaches, see this previous blog post.)

We turn to the details. Let ${V_n}$ be the space of Hermitian ${n \times n}$ matrices, then the distribution ${\mu_{M_n}}$ of a GUE matrix ${M_n}$ is a absolutely continuous probability measure on ${V_n}$, which can be written using the definition of GUE as

$\displaystyle \mu_{M_n} = C_n (\prod_{1 \leq i < j \leq n} e^{-|\xi_{ij}|^2}) (\prod_{1 \leq i \leq n} e^{-|\xi_{ii}|^2/2})\ dM_n$

where ${dM_n}$ is Lebesgue measure on ${V}$, ${\xi_{ij}}$ are the coordinates of ${M_n}$, and ${C_n}$ is a normalisation constant (the exact value of which depends on how one normalises Lebesgue measure on ${V}$). We can express this more compactly as

$\displaystyle \mu_{M_n} = C_n e^{- \hbox{tr}(M_n^2) / 2}\ dM_n.$

Expressed this way, it is clear that the GUE ensemble is invariant under conjugations ${M_n \mapsto U M_n U^{-1}}$ by any unitary matrix.

Let ${D}$ be the diagonal matrix whose entries ${\lambda_1 \geq \ldots \geq \lambda_n}$ are the eigenvalues of ${M_n}$ in descending order. Then we have ${M_n = U D U^{-1}}$ for some unitary matrix ${U \in U(n)}$. The matirx ${U}$ is not uniquely determined; if ${R}$ is diagonal unitary matrix, then ${R}$ commutes with ${D}$, and so one can freely replace ${U}$ with ${UR}$. On the other hand, if the eigenvalues of ${M}$ are simple, then the diagonal matrices are the only matrices that commute with ${D}$, and so this freedom to right-multiply ${U}$ by diagonal unitaries is the only failure of uniqueness here. And in any case, from the unitary invariance of GUE, we see that even after conditioning on ${D}$, we may assume without loss of generality that ${U}$ is drawn from the invariant Haar measure on ${U(n)}$. In particular, ${U}$ and ${D}$ can be taken to be independent.

Fix a diagonal matrix ${D_0 = \hbox{diag}(\lambda_1^0,\ldots,\lambda_n^0)}$ for some ${\lambda_1^0 > \ldots > \lambda_n^0}$, let ${\epsilon > 0}$ be extremely small, and let us compute the probability

$\displaystyle \mathop{\bf P}( \| M_n - D_0 \|_F \leq \epsilon ) \ \ \ \ \ (2)$

that ${M_n}$ lies within ${\epsilon}$ of ${D_0}$ in the Frobenius norm. On the one hand, the probability density of ${M_n}$ is proportional to

$\displaystyle e^{-\hbox{tr}(D_0^2)/2} = e^{-|\lambda^0|^2/2}$

near ${D_0}$ (where we write ${\lambda^0 := (\lambda_1^0,\ldots,\lambda_n^0)}$) and the volume of a ball of radius ${\epsilon}$ in the ${n^2}$-dimensional space ${V_n}$ is proportional to ${\epsilon^{n^2}}$, so (2) is equal to

$\displaystyle (C'_n + o(1)) \epsilon^{n^2} e^{-\hbox{tr}(D_0^2)/2} \ \ \ \ \ (3)$

for some constant ${C'_n > 0}$ depending only on ${n}$, where ${o(1)}$ goes to zero as ${\epsilon \rightarrow 0}$ (keeping ${n}$ and ${D_0}$ fixed). On the other hand, if ${\|M_n - D_0\|_F \leq \epsilon}$, then by the Weyl inequality (or Hoffman-Weilandt inequality) we have ${D = D_0 + O(\epsilon)}$ (we allow implied constants here to depend on ${n}$ and on ${D_0}$). This implies ${UDU^{-1} = D + O(\epsilon)}$, thus ${UD - DU = O(\epsilon)}$. As a consequence we see that the off-diagonal elements of ${U}$ are of size ${O(\epsilon)}$. We can thus use the inverse function theorem in this local region of parameter space and make the ansatz

$\displaystyle D = D_0 + \epsilon E; \quad U = \exp( \epsilon S ) R$

where ${E}$ is a bounded diagonal matrix, ${R}$ is a diagonal unitary matrix, and ${S}$ is a bounded skew-adjoint matrix with zero diagonal. (Note here the emergence of the freedom to right-multiply ${U}$ by diagonal unitaries.) Note that the map ${(R,S) \mapsto \exp( \epsilon S ) R}$ has a non-degenerate Jacobian, so the inverse function theorem applies to uniquely specify ${R, S}$ (and thus ${E}$) from ${U, D}$ in this local region of parameter space.

Conversely, if ${D, U}$ take the above form, then we can Taylor expand and conclude that

$\displaystyle M_n = UDU^* = D_0 + \epsilon E + \epsilon (SD_0 - D_0S) + O(\epsilon^2)$

and so

$\displaystyle \| M_n - D_0 \|_F = \epsilon \| E + (SD_0 - D_0S)\|_F + O(\epsilon^2).$

We can thus bound (2) from above and below by expressions of the form

$\displaystyle \mathop{\bf P}( \| E + (SD_0 - D_0S)\|_F \leq 1 + O(\epsilon) ). \ \ \ \ \ (4)$

As ${U}$ is distributed using Haar measure on ${U(n)}$, ${S}$ is (locally) distributed using ${\epsilon^{n^2-n}}$ times a constant multiple of Lebesgue measure on the space ${W}$ of skew-adjoint matrices with zero diagonal, which has dimension ${n^2-n}$. Meanwhile, ${E}$ is distributed using ${(\rho_n(\lambda^0)+o(1)) \epsilon^{n}}$ times Lebesgue measure on the space of diagonal elements. Thus we can rewrite (4) as

$\displaystyle C''_n \epsilon^{n^2} (\rho_n(\lambda^0)+o(1)) \int\int_{\| E + (SD_0 - D_0S)\|_F \leq 1 + O(\epsilon)}\ dE dS$

where ${dE}$ and ${dS}$ denote Lebesgue measure and ${C''_n > 0}$ depends only on ${n}$.

Observe that the map ${S \mapsto SD_0-D_0 S}$ dilates the (complex-valued) ${ij}$ entry of ${S}$ by ${\lambda^0_j-\lambda^0_i}$, and so the Jacobian of this map is ${\prod_{1 \leq i < j \leq n} |\lambda^0_j-\lambda^0_i|^2 = |\Delta_n(\lambda^0)|^2}$. Applying the change of variables, we can express the above as

$\displaystyle C''_n \epsilon^{n^2} \frac{\rho_n(\lambda^0)+o(1)}{|\Delta_n(\lambda^0)|^2} \int\int_{\| E + S\|_F \leq 1 + O(\epsilon)}\ dE dS.$

The integral here is of the form ${C'''_n + O(\epsilon)}$ for some other constant ${C'''_n > 0}$. Comparing this formula with (3) we see that

$\displaystyle \rho_n(\lambda^0)+o(1) = C''''_n e^{-|\lambda^0|^2/2} \Delta_n(\lambda^0)|^2 + o(1)$

for yet another constant ${C''''_n > 0}$. Sending ${\epsilon \rightarrow 0}$ we recover an exact formula

$\displaystyle \rho_n(\lambda)+o(1) = C''''_n e^{-|\lambda|^2/2} |\Delta_n(\lambda)|^2$

when ${\lambda}$ is simple. Since almost all Hermitian matrices have simple spectrum (see Exercise 10 of Notes 3a), this gives the full spectral distribution of GUE, except for the issue of the unspecified constant.

Remark 1 In principle, this method should also recover the explicit normalising constant ${\frac{1}{(2\pi)^{n/2}}}$ in (1), but to do this it appears one needs to understand the volume of the fundamental domain of ${U(n)}$ with respect to the logarithm map, or equivalently to understand the volume of the unit ball of Hermitian matrices in the operator norm. I do not know of a simple way to compute this quantity (though it can be inferred from (1) and the above analysis). One can also recover the normalising constant through the machinery of determinantal processes, see below.

Remark 2 The above computation can be generalised to other ${U(n)}$-conjugation-invariant ensembles ${M_n}$ whose probability distribution is of the form

$\displaystyle \mu_{M_n} = C_n e^{- \hbox{tr} V(M_n)}\ dM_n$

for some potential function ${V: {\bf R} \rightarrow {\bf R}}$ (where we use the spectral theorem to define ${V(M_n)}$), yielding a density function for the spectrum of the form

$\displaystyle \rho_n(\lambda) = C'_n e^{- \sum_{j=1}^n V(\lambda_j)} |\Delta_n(\lambda)|^2.$

Given suitable regularity conditions on ${V}$, one can then generalise many of the arguments in these notes to such ensembles. See this book by Deift for details.

— 2. The spectrum of gaussian matrices —

The above method also works for gaussian matrices ${G}$, as was first observed by Dyson (though the final formula was first obtained by Ginibre, using a different method). Here, the density function is given by

$\displaystyle C_n e^{-\hbox{tr}( GG^*)} dG = C_n e^{-\|G\|_F^2} dG \ \ \ \ \ (5)$

where ${C_n > 0}$ is a constant and ${dG}$ is Lebesgue measure on the space ${M_n({\bf C})}$ of all complex ${n \times n}$ matrices. This is invariant under both left and right multiplication by unitary matrices, so in particular is invariant under unitary conjugations as before.

This matrix ${G}$ has ${n}$ complex (generalised) eigenvalues ${\sigma(G) = \{\lambda_1,\ldots,\lambda_n\}}$, which are usually distinct:

Exercise 1 Let ${n \geq 2}$. Show that the space of matrices in ${M_n({\bf C})}$ with a repeated eigenvalue has codimension ${2}$.

Unlike the Hermitian situation, though, there is no natural way to order these ${n}$ complex eigenvalues. We will thus consider all ${n!}$ possible permutations at once, and define the spectral density function ${\rho_n(\lambda_1,\ldots,\lambda_n)}$ of ${G}$ by duality and the formula

$\displaystyle \int_{{\bf C}^n} F(\lambda) \rho_n(\lambda)\ d\lambda := \mathop{\bf E} \sum_{\{\lambda_1,\ldots,\lambda_n\} = \sigma(G)} F(\lambda_1,\ldots,\lambda_n)$

for all test functions ${F}$. By the Riesz representation theorem, this uniquely defines ${\rho_n}$ (as a distribution, at least), although the total mass of ${\rho_n}$ is ${n!}$ rather than ${1}$ due to the ambiguity in the spectrum.

Now we compute ${\rho_n}$ (up to constants). In the Hermitian case, the key was to use the factorisation ${M_n = UDU^{-1}}$. This particular factorisation is of course unavailable in the non-Hermitian case. However, if the non-Hermitian matrix ${G}$ has simple spectrum, it can always be factored instead as ${G = UTU^{-1}}$, where ${U}$ is unitary and ${T}$ is upper triangular. Indeed, if one applies the Gram-Schmidt process to the eigenvectors of ${G}$ and uses the resulting orthonormal basis to form ${U}$, one easily verifies the desired factorisation. Note that the eigenvalues of ${G}$ are the same as those of ${T}$, which in turn are just the diagonal entries of ${T}$.

Exercise 2 Show that this factorisation is also available when there are repeated eigenvalues. (Hint: use the Jordan normal form.)

To use this factorisation, we first have to understand how unique it is, at least in the generic case when there are no repeated eigenvalues. As noted above, if ${G = UTU^{-1}}$, then the diagonal entries of ${T}$ form the same set as the eigenvalues of ${G}$.

Now suppose we fix the diagonal ${\lambda_1,\ldots,\lambda_n}$ of ${T}$, which amounts to picking an ordering of the ${n}$ eigenvalues of ${G}$. The eigenvalues of ${T}$ are ${\lambda_1,\ldots,\lambda_n}$, and furthermore for each ${1 \leq j \leq n}$, the eigenvector of ${T}$ associated to ${\lambda_j}$ lies in the span of the last ${n-j+1}$ basis vectors ${e_j,\ldots,e_n}$ of ${{\bf C}^n}$, with a non-zero ${e_j}$ coefficient (as can be seen by Gaussian elimination or Cramer’s rule). As ${G=UTU^{-1}}$ with ${U}$ unitary, we conclude that for each ${1 \leq j \leq n}$, the ${j^{th}}$ column of ${U}$ lies in the span of the eigenvectors associated to ${\lambda_j,\ldots,\lambda_n}$. As these columns are orthonormal, they must thus arise from applying the Gram-Schmidt process to these eigenvectors (as discussed earlier). This argument also shows that once the diagonal entries ${\lambda_1,\ldots,\lambda_n}$ of ${T}$ are fixed, each column of ${U}$ is determined up to rotation by a unit phase. In other words, the only remaining freedom is to replace ${U}$ by ${UR}$ for some unit diagonal matrix ${R}$, and then to replace ${T}$ by ${R^{-1}TR}$ to counterbalance this change of ${U}$.

To summarise, the factorisation ${G = UTU^{-1}}$ is unique up to specifying an enumeration ${\lambda_1,\ldots,\lambda_n}$ of the eigenvalues of ${G}$ and right-multiplying ${U}$ by diagonal unitary matrices, and then conjugating ${T}$ by the same matrix. Given a matrix ${G}$, we may apply these symmetries randomly, ending up with a random enumeration ${\lambda_1,\ldots,\lambda_n}$ of the eigenvalues of ${G}$ (whose distribution invariant with respect to permutations) together with a random factorisation ${UTU^{-1}}$ such that ${T}$ has diagonal entries ${\lambda_1,\ldots,\lambda_n}$ in that order, and the distribution of ${T}$ is invariant under conjugation by diagonal unitary matrices. Also, since ${G}$ is itself invariant under unitary conjugations, we may also assume that ${U}$ is distributed uniformly according to the Haar measure of ${U(n)}$, and independently of ${T}$.

To summarise, the gaussian matrix ensemble ${G}$, together with a randomly chosen enumeration ${\lambda_1,\ldots,\lambda_n}$ of the eigenvalues, can almost surely be factorised as ${UTU^{-1}}$, where ${T = ( t_{ij} )_{1 \leq i \leq j \leq n}}$ is an upper-triangular matrix with diagonal entries ${\lambda_1,\ldots,\lambda_n}$, distributed according to some distribution

$\displaystyle \psi( (t_{ij})_{1 \leq i \leq j \leq n} )\ \prod_{1 \leq i \leq j \leq n} dt_{ij}$

which is invariant with respect to conjugating ${T}$ by diagonal unitary matrices, and ${U}$ is uniformly distributed according to the Haar measure of ${U(n)}$, independently of ${T}$.

Now let ${T_0 = ( t_{ij}^0 )_{1 \leq i \leq j \leq n}}$ be an upper triangular matrix with complex entries whose entries ${t_{11}^0,\ldots,t_{nn}^0 \in {\bf C}}$ are distinct. As in the previous section, we consider the probability

$\displaystyle \mathop{\bf P}( \| G - T_0 \|_F \leq \epsilon ) . \ \ \ \ \ (6)$

On the one hand, since the space ${M_n({\bf C})}$ of complex ${n \times n}$ matrices has ${2n^2}$ real dimensions, we see from (9) that this expression is equal to

$\displaystyle (C'_n+o(1)) e^{-\|T_0\|_F^2} \epsilon^{2n^2} \ \ \ \ \ (7)$

for some constant ${C'_n > 0}$.

Now we compute (6) using the factorisation ${G = UTU^{-1}}$. Suppose that ${\|G-T_0\|_F \leq \epsilon}$, so ${G = T_0+O(\epsilon)}$ As the eigenvalues of ${T_0}$ are ${t_{11}^0,\ldots,t_{nn}^0}$, which are assumed to be distinct, we see (from the inverse function theorem) that for ${\epsilon}$ small enough, ${G}$ has eigenvalues ${t_{11}^0 +O(\epsilon), \ldots, t_{nn}^0 + O(\epsilon)}$. With probability ${1/n!}$, the diagonal entries of ${T}$ are thus ${t_{11}^0 +O(\epsilon), \ldots, t_{nn}^0 + O(\epsilon)}$ (in that order). We now restrict to this event (the ${1/n!}$ factor will eventually be absorbed into one of the unspecified constants).

Let ${u^0_1,\ldots,u^0_n}$ be eigenvector of ${T_0}$ associated to ${t_{11}^0,\ldots,t_{nn}^0}$, then the Gram-Schmidt process applied to ${u_1,\ldots,u_n}$ (starting at ${u^0_n}$ and working backwards to ${u^0_1}$) gives the standard basis ${e_1,\ldots,e_n}$ (in reverse order). By the inverse function theorem, we thus see that we have eigenvectors ${u_1 = u^0_1+O(\epsilon),\ldots,u_n=u^0_n+O(\epsilon)}$ of ${G}$, which when the Gram-Schmidt process is applied, gives a perturbation ${e_1+O(\epsilon),\ldots,e_n+O(\epsilon)}$ in reverse order. This gives a factorisation ${G=UTU^{-1}}$ in which ${U = I + O(\epsilon)}$, and hence ${T = T_0+O(\epsilon)}$. This is however not the most general factorisation available, even after fixing the diagonal entries of ${T}$, due to the freedom to right-multiply ${U}$ by diagonal unitary matrices ${R}$. We thus see that the correct ansatz here is to have

$\displaystyle U = R + O(\epsilon); \quad T = R^{-1} T_0 R + O(\epsilon)$

for some diagonal unitary matrix ${R}$.

In analogy with the GUE case, we can use the inverse function theorem and make the more precise ansatz

$\displaystyle U = \exp(\epsilon S) R; \quad T = R^{-1} (T_0 + \epsilon E) R$

where ${S}$ is skew-Hermitian with zero diagonal and size ${O(1)}$, ${R}$ is diagonal unitary, and ${E}$ is an upper triangular matrix of size ${O(1)}$. From the invariance ${U \mapsto UR; T \mapsto R^{-1} TR}$ we see that ${R}$ is distributed uniformly across all diagonal unitaries. Meanwhile, from the unitary conjugation invariance, ${S}$ is distributed according to a constant multiple of ${\epsilon^{n^2-n}}$ times Lebesgue measure ${dS}$ on the ${n^2-n}$-dimensional space of skew Hermitian matrices with zero diagonal; and from the definition of ${\psi}$, ${E}$ is distributed according to a constant multiple of the measure

$\displaystyle (1+o(1)) \epsilon^{n^2+n} \psi(T_0)\ dE,$

where ${dE}$ is Lebesgue measure on the ${n^2+n}$-dimensional space of upper-triangular matrices. Furthermore, the invariances ensure that the random variables ${S, R, E}$ are distributed independently. Finally, we have

$\displaystyle G = UTU^{-1} = \exp(\epsilon S) (T_0 + \epsilon E) \exp(-\epsilon S).$

Thus we may rewrite (6) as

$\displaystyle (C''_n \psi(T_0)+o(1))\epsilon^{2n^2} \int\int_{\|\exp(\epsilon S) (T_0 + \epsilon E) \exp(-\epsilon S) - T_0\|_F \leq \epsilon} dS dE \ \ \ \ \ (8)$

for some ${C''_n>0}$ (the ${R}$ integration being absorbable into this constant ${C''_n}$). We can Taylor expand

$\displaystyle \exp(\epsilon S) (T_0 + \epsilon E) \exp(-\epsilon S) = T_0 + \epsilon (E + ST_0 - T_0S) + O(\epsilon^2)$

and so we can bound (8) above and below by expressions of the form

$\displaystyle (C''_n \psi(T_0)+o(1))\epsilon^{2n^2} \int\int_{\|E + ST_0 - T_0 S\|_F \leq 1+O(\epsilon)} dS dE.$

The Lebesgue measure ${dE}$ is invariant under translations by upper triangular matrices, so we may rewrite the above expression as

$\displaystyle (C''_n \psi(T_0)+o(1))\epsilon^{2n^2} \int\int_{\|E + \pi(ST_0 - T_0 S)\|_F \leq 1+O(\epsilon)} dS dE, \ \ \ \ \ (9)$

where ${\pi(ST_0 - T_0 S)}$ is the strictly lower triangular component of ${ST_0-T_0S}$.

The next step is to make the (linear) change of variables ${V := \pi(ST_0-T_0 S)}$. We check dimensions: ${S}$ ranges in the space ${S}$ of skew-adjoint Hermitian matrices with zero diagonal, which has dimension ${(n^2-n)/2}$, as does the space of strictly lower-triangular matrices, which is where ${V}$ ranges. So we can in principle make this change of variables, but we first have to compute the Jacobian of the transformation (and check that it is non-zero). For this, we switch to coordinates. Write ${S = (s_{ij})_{1 \leq i, j \leq n}}$ and ${V = (v_{ij})_{1 \leq j < i \leq n}}$. In coordinates, the equation ${V=\pi(ST_0-T_0S)}$ becomes

$\displaystyle v_{ij} = \sum_{k=1}^j s_{ik} t_{kj}^0 - \sum_{k=i}^n t_{ik}^0 s_{kj}$

or equivalently

$\displaystyle v_{ij} = (t_{jj}^0-t_{ii}^0) s_{ij} + \sum_{k=1}^{j-1} t_{kj}^0 s_{ik}- \sum_{k=i+1}^n t_{ik}^0 s_{kj}.$

Thus for instance

$\displaystyle v_{n1} = (t^0_{11}-t^0_{nn}) s_{n1}$

$\displaystyle v_{n2} = (t^0_{22}-t^0_{nn}) s_{n2} + t_{12}^0 s_{n1}$

$\displaystyle v_{(n-1)1} = (t^0_{11} - t^0_{(n-1)(n-1)}) s_{(n-1)1} - t_{(n-1)n}^0 s_{n1}$

$\displaystyle v_{n3} = (t^0_{33}-t^0_{nn}) s_{n3} + t_{13}^0 s_{n1} + t_{23}^0 s_{n2}$

$\displaystyle v_{(n-1)2} = (t^0_{22}-t^0_{(n-1)(n-1)}) s_{(n-1)2} +t_{12}^0 s_{(n-1)1} - t_{(n-1)n}^0 s_{n2}$

$\displaystyle v_{(n-2)1} = (t^0_{11}-t^0_{(n-2)(n-2)}) s_{(n-2)1} - t_{(n-2)(n-1)}^0 s_{(n-1)1} - t_{(n-2)n}^0 s_{n1}$

etc. We then observe that the transformation matrix from ${s_{n1}, s_{n2}, s_{(n-1)1},\ldots}$ to ${v_{n1}, v_{n2}, v_{(n-1)1}, \ldots}$ is triangular, with diagonal entries given by ${t^0_{jj}-t^0_{ii}}$ for ${1 \leq j < i \leq n}$. The Jacobian of the (complex-linear) map ${S \mapsto V}$ is thus given by

$\displaystyle |\prod_{1 \leq j < i \leq n} t^0_{jj}-t^0_{ii}|^2 = |\Delta( t^0_{11},\ldots,t^0_{nn})|^2$

which is non-zero by the hypothesis that the ${t_0^{11},\ldots,t_0^{nn}}$ are distinct. We may thus rewrite (9) as

$\displaystyle \frac{C''_n \psi(T_0)+o(1)}{|\Delta( t^0_{11},\ldots,t^0_{nn})|^2} \epsilon^{2n^2}\int\int_{\|E + V\|_F \leq 1+O(\epsilon)} dS dV$

where ${dV}$ is Lebesgue measure on strictly lower-triangular matrices. The integral here is equal to ${C'''_n + O(\epsilon)}$ for some constant ${C'''_n}$. Comparing this with (6), cancelling the factor of ${\epsilon^{2n^2}}$, and sending ${\epsilon \rightarrow 0}$, we obtain the formula

$\displaystyle \psi( (t^0_{ij})_{1 \leq i \leq j \leq n} ) = C''''_n |\Delta( t^0_{11},\ldots,t^0_{nn})|^2 e^{-\|T_0\|_F^2}$

for some constant ${C''''_n > 0}$. We can expand

$\displaystyle e^{-\|T_0\|_F^2} = \prod_{1 \leq i \leq j \leq n} e^{-|t_{ij}^0|^2}.$

If we integrate out the off-diagonal variables ${t^0_{ij}}$ for ${1 \leq i < j \leq n}$, we see that the density function for the diagonal entries ${(\lambda_1,\ldots,\lambda_n)}$ of ${T}$ is proportional to

$\displaystyle |\Delta(\lambda_1,\ldots,\lambda_n)|^2 e^{-\sum_{j=1}^n |\lambda_j|^2}.$

Since these entries are a random permutation of the eigenvalues of ${G}$, we conclude the Ginibre formula

$\displaystyle \rho_n(\lambda_1,\ldots,\lambda_n) = c_n |\Delta(\lambda_1,\ldots,\lambda_n)|^2 e^{-\sum_{j=1}^n |\lambda_j|^2} \ \ \ \ \ (10)$

for the joint density of the eigenvalues of a gaussian random matrix, where ${c_n > 0}$ is a constant.

Remark 3 Given that (1) can be derived using Dyson Brownian motion, it is natural to ask whether (10) can be derived by a similar method. It seems that in order to do this, one needs to consider a Dyson-like process not just on the eigenvalues ${\lambda_1,\ldots,\lambda_n}$, but on the entire triangular matrix ${T}$ (or more precisely, on the moduli space formed by quotienting out the action of conjugation by unitary diagonal matrices). Unfortunately the computations seem to get somewhat complicated, and we do not present them here.

— 3. Mean field approximation —

We can use the formula (1) for the joint distribution to heuristically derive the semicircular law, as follows.

It is intuitively plausible that the spectrum ${(\lambda_1,\ldots,\lambda_n)}$ should concentrate in regions in which ${\rho_n(\lambda_1,\ldots,\lambda_n)}$ is as large as possible. So it is now natural to ask how to optimise this function. Note that the expression in (1) is non-negative, and vanishes whenever two of the ${\lambda_i}$ collide, or when one or more of the ${\lambda_i}$ go off to infinity, so a maximum should exist away from these degenerate situations.

We may take logarithms and write

$\displaystyle - \log \rho_n(\lambda_1,\ldots,\lambda_n) = \sum_{j=1}^n \frac{1}{2} |\lambda_j|^2 + \sum\sum_{i \neq j} \log \frac{1}{|\lambda_i-\lambda_j|} + C \ \ \ \ \ (11)$

where ${C = C_n}$ is a constant whose exact value is not of importance to us. From a mathematical physics perspective, one can interpret (11) as a Hamiltonian for ${n}$ particles at positions ${\lambda_1,\ldots,\lambda_n}$, subject to a confining harmonic potential (these are the ${\frac{1}{2} |\lambda_j|^2}$ terms) and a repulsive logarithmic potential between particles (these are the ${\frac{1}{|\lambda_i-\lambda_j|}}$ terms).

Our objective is now to find a distribution of ${\lambda_1,\ldots,\lambda_n}$ that minimises this expression.

We know from previous notes that the ${\lambda_i}$ should be have magnitude ${O(\sqrt{n})}$. Let us then heuristically make a mean field approximation, in that we approximate the discrete spectral measure ${\frac{1}{n} \sum_{j=1}^n \delta_{\lambda_j/\sqrt{n}}}$ by a continuous probability measure ${\rho(x)\ dx}$. (Secretly, we know from the semi-circular law that we should be able to take ${\rho = \frac{1}{2\pi} (4-x^2)_+^{1/2}}$, but pretend that we do not know this fact yet.) Then we can heuristically approximate (11) as

$\displaystyle n^2 ( \int_{\bf R} \frac{1}{2} x^2 \rho(x)\ dx + \int_{\bf R} \int_{\bf R} \log \frac{1}{|x-y|} \rho(x) \rho(y)\ dx dy ) + C'_n$

and so we expect the distribution ${\rho}$ to minimise the functional

$\displaystyle \int_{\bf R} \frac{1}{2} x^2 \rho(x)\ dx + \int_{\bf R} \int_{\bf R} \log \frac{1}{|x-y|} \rho(x) \rho(y)\ dx dy. \ \ \ \ \ (12)$

One can compute the Euler-Lagrange equations of this functional:

Exercise 3 Working formally, and assuming that ${\rho}$ is a probability measure that minimises (12), argue that

$\displaystyle \frac{1}{2} x^2 + 2 \int_{\bf R} \log \frac{1}{|x-y|} \rho(y)\ dy = C$

for some constant ${C}$ and all ${x}$ in the support of ${\rho}$. For all ${x}$ outside of the support, establish the inequality

$\displaystyle \frac{1}{2} x^2 + 2 \int_{\bf R} \log \frac{1}{|x-y|} \rho(y)\ dy \geq C.$

There are various ways we can solve this equation for ${\rho}$; we sketch here a complex-analytic method. Differentiating in ${x}$, we formally obtain

$\displaystyle x - 2 p.v. \int_{\bf R} \frac{1}{x-y} \rho(y)\ dy = 0$

on the support of ${\rho}$. But recall that if we let

$\displaystyle s(z) := \int_{\bf R} \frac{1}{y-z} \rho(y)\ dy$

be the Stieltjes transform of the probability measure ${\rho(x)\ dx}$, then we have

$\displaystyle \hbox{Im}(s(x+i0^+)) = \pi \rho(x)$

and

$\displaystyle \hbox{Re}(s(x+i0^+)) = - p.v. \int_{\bf R} \frac{1}{x-y} \rho(y)\ dy.$

We conclude that

$\displaystyle (x + 2 \hbox{Re}(s(x+i0^+)) \hbox{Im}(s(x+i0^+))) = 0$

for all ${x}$, which we rearrange as

$\displaystyle \hbox{Im}( s^2(x+i0^+) + x s(x+i0^+) ) = 0.$

This makes the function ${f(z) = s^2(z) + z s(z)}$ entire (it is analytic in the upper half-plane, obeys the symmetry ${f(\overline{z}) = \overline{f(z)}}$, and has no jump across the real line). On the other hand, as ${s(z) = \frac{-1+o(1)}{z}}$ as ${z \rightarrow \infty}$, ${f}$ goes to ${-1}$ at infinity. Applying Liouville’s theorem, we conclude that ${f}$ is constant, thus we have the familiar equation

$\displaystyle s^2 + zs = -1$

which can then be solved to obtain the semi-circular law as in previous notes.

Remark 4 Recall from Notes 3b that Dyson Brownian motion can be used to derive the formula (1). One can then interpret the Dyson Brownian motion proof of the semi-circular law for GUE in Notes 4 as a rigorous formalisation of the above mean field approximation heuristic argument.

One can perform a similar heuristic analysis for the spectral measure ${\mu_G}$ of a random gaussian matrix, giving a description of the limiting density:

Exercise 4 Using heuristic arguments similar to those above, argue that ${\mu_G}$ should be close to a continuous probability distribution ${\rho(z)\ dz}$ obeying the equation

$\displaystyle |z|^2 + \int_{\bf C} \log \frac{1}{|z-w|} \rho(w)\ dw = C$

on the support of ${\rho}$, for some constant ${C}$, with the inequality

$\displaystyle |z|^2 + \int_{\bf C} \log \frac{1}{|z-w|} \rho(w)\ dw \geq C. \ \ \ \ \ (13)$

Using the Newton potential ${\frac{1}{2\pi} \log |z|}$ for the fundamental solution of the two-dimensional Laplacian ${-\partial_x^2 - \partial_y^2}$, conclude (non-rigorously) that ${\rho}$ is equal to ${\frac{1}{\pi}}$ on its support.

Also argue that ${\rho}$ should be rotationally symmetric. Use (13) and Green’s formula to argue why the support of ${\rho}$ should be simply connected, and then conclude (again non-rigorously) the circular law

$\displaystyle \mu_G \approx \frac{1}{\pi} 1_{|z| \leq 1}\ dz. \ \ \ \ \ (14)$

We will see more rigorous derivations of the circular law later in these notes, and also in subsequent notes.

— 4. Determinantal form of the GUE spectral distribution —

In a previous section, we showed (up to constants) that the density function ${\rho_n(\lambda_1,\ldots,\lambda_n)}$ for the eigenvalues ${\lambda_1 \geq \ldots \geq \lambda_n}$ of GUE was given by the formula (1).

As is well known, the Vandermonde determinant ${\Delta(\lambda_1,\ldots,\lambda_n)}$ that appears in (1) can be expressed up to sign as a determinant of an ${n \times n}$ matrix, namely the matrix ${(\lambda_i^{j-1})_{1 \leq i,j \leq n}}$. Indeed, this determinant is clearly a polynomial of degree ${n(n-1)/2}$ in ${\lambda_1,\ldots,\lambda_n}$ which vanishes whenever two of the ${\lambda_i}$ agree, and the claim then follows from the factor theorem (and inspecting a single coefficient of the Vandermonde determinant, e.g. the ${\prod_{j=1}^n \lambda_j^{j-1}}$ coefficient, to get the sign).

We can square the above fact (or more precisely, multiply the above matrix matrix by its adjoint) and conclude that ${|\Delta(\lambda_1,\ldots,\lambda_n)|^2}$ is the determinant of the matrix

$\displaystyle ( \sum_{k=0}^{n-1} \lambda_i^k \lambda_j^k )_{1 \leq i,j \leq n}.$

More generally, if ${P_0(x),\ldots,P_{n-1}(x)}$ are any sequence of polynomials, in which ${P_i(x)}$ has degree ${i}$, then we see from row operations that the determinant of

$\displaystyle (P_{j-1}(\lambda_i))_{1 \leq i,j \leq n}$

is a non-zero constant multiple of ${\Delta(\lambda_1,\ldots,\lambda_n)}$ (with the constant depending on the leading coefficients of the ${P_i}$), and so the determinant of

$\displaystyle ( \sum_{k=0}^{n-1} P_k(\lambda_i) P_k(\lambda_j) )_{1 \leq i,j \leq n}$

is a non-zero constant multiple of ${|\Delta(\lambda_1,\ldots,\lambda_n)|^2}$. Comparing this with (1), we obtain the formula

$\displaystyle \rho_n(\lambda) = C \det( \sum_{k=0}^{n-1} P_k(\lambda_i) e^{-\lambda_i^2/4} P_k(\lambda_j) e^{-\lambda_j^2/4})_{1 \leq i,j \leq n}$

for some non-zero constant ${C}$.

This formula is valid for any choice of polynomials ${P_i}$ of degree ${i}$. But the formula is particularly useful when we set ${P_i}$ equal to the (normalised) Hermite polynomials, defined by applying the Gram-Schmidt process in ${L^2({\bf R})}$ to the polynomials ${x^i e^{-x^2/4}}$ for ${i=0,\ldots,n-1}$ to yield ${P_i(x) e^{-x^2/4}}$. (Equivalently, the ${P_i}$ are the orthogonal polynomials associated to the measure ${e^{-x^2/2}\ dx}$.) In that case, the expression

$\displaystyle K_n(x,y) := \sum_{k=0}^{n-1} P_k(x) e^{-x^2/4} P_k(y) e^{-y^2/4} \ \ \ \ \ (15)$

becomes the integral kernel of the orthogonal projection ${\pi_{V_n}}$ operator in ${L^2({\bf R})}$ to the span of the ${x^i e^{-x^2/4}}$, thus

$\displaystyle \pi_{V_n} f(x) = \int_{\bf R} K_n(x,y) f(y)\ dy$

for all ${f \in L^2({\bf R})}$, and so ${\rho_n(\lambda)}$ is now a constant multiple of

$\displaystyle \det( K_n(\lambda_i, \lambda_j) )_{1 \leq i,j \leq n}.$

The reason for working with orthogonal polynomials is that we have the trace identity

$\displaystyle \int_{\bf R} K_n(x,x)\ dx = \hbox{tr}(\pi_{V_n}) = n \ \ \ \ \ (16)$

and the reproducing formula

$\displaystyle K_n(x,y) = \int_{\bf R} K_n(x,z) K_n(z,y)\ dz \ \ \ \ \ (17)$

which reflects the identity ${\pi_{V_n} = \pi_{V_n}^2}$. These two formulae have an important consequence:

Lemma 1 (Determinantal integration formula) Let ${K_n: {\bf R} \times {\bf R} \rightarrow {\bf R}}$ be any symmetric rapidly decreasing function obeying (16), (17). Then for any ${k \geq 0}$, one has

$\displaystyle \int_{\bf R} \det( K_n(\lambda_i, \lambda_j) )_{1 \leq i,j \leq k+1}\ d\lambda_{k+1} = (n-k) \det( K_n(\lambda_i, \lambda_j) )_{1 \leq i,j \leq k}. \ \ \ \ \ (18)$

Remark 5 This remarkable identity is part of the beautiful algebraic theory of determinantal processes, which I discuss further in this blog post.

Proof: We induct on ${k}$. When ${k=0}$ this is just (16). Now assume that ${k \geq 1}$ and that the claim has already been proven for ${k-1}$. We apply cofactor expansion to the bottom row of the determinant ${\det( K_n(\lambda_i, \lambda_j) )_{1 \leq i,j \leq k+1}}$. This gives a principal term

$\displaystyle \det( K_n(\lambda_i, \lambda_j) )_{1 \leq i,j \leq k} K_n(\lambda_{k+1},\lambda_{k+1}) \ \ \ \ \ (19)$

plus a sum of ${k}$ additional terms, the ${l^{th}}$ term of which is of the form

$\displaystyle (-1)^{k+1-l} K_n(\lambda_l,\lambda_{k+1}) \det( K_n(\lambda_i, \lambda_j) )_{1 \leq i \leq k; 1 \leq j \leq k+1; j \neq l}. \ \ \ \ \ (20)$

Using (16), the principal term (19) gives a contribution of ${n \det( K_n(\lambda_i, \lambda_j) )_{1 \leq i,j \leq k}}$ to (18). For each nonprincipal term (20), we use the multilinearity of the determinant to absorb the ${K_n(\lambda_l,\lambda_{k+1})}$ term into the ${j=k+1}$ column of the matrix. Using (17), we thus see that the contribution of (20) to (18) can be simplified as

$\displaystyle (-1)^{k+1-l} \det( ( K_n(\lambda_i, \lambda_j) )_{1 \leq i \leq k; 1 \leq j \leq k; j \neq l}, (K_n(\lambda_i,\lambda_l))_{1 \leq i\leq k} )$

which after row exchange, simplifies to ${-\det( K_n(\lambda_i, \lambda_j) )_{1 \leq i,j \leq k}}$. The claim follows. $\Box$

In particular, if we iterate the above lemma using the Fubini-Tonelli theorem, we see that

$\displaystyle \int_{{\bf R}^n} \det( K_n(\lambda_i, \lambda_j) )_{1 \leq i,j \leq n}\ d\lambda_1 \ldots d\lambda_n = n!.$

On the other hand, if we extend the probability density function ${\rho_n(\lambda_1,\ldots,\lambda_n)}$ symmetrically from the Weyl chamber ${{\bf R}^n_{\geq}}$ to all of ${{\bf R}^n}$, its integral is also ${n!}$. Since ${\det( K_n(\lambda_i, \lambda_j) )_{1 \leq i,j \leq n}}$ is clearly symmetric in the ${\lambda_1,\ldots,\lambda_n}$, we can thus compare constants and conclude the Gaudin-Mehta formula

$\displaystyle \rho_n(\lambda_1,\ldots,\lambda_n) = \det( K_n(\lambda_i, \lambda_j) )_{1 \leq i,j \leq n}.$

More generally, if we define ${\rho_k: {\bf R}^k \rightarrow {\bf R}^+}$ to be the function

$\displaystyle \rho_k(\lambda_1,\ldots,\lambda_k) = \det( K_n(\lambda_i, \lambda_j) )_{1 \leq i,j \leq k}, \ \ \ \ \ (21)$

then the above formula shows that ${\rho_k}$ is the ${k}$-point correlation function for the spectrum, in the sense that

$\displaystyle \int_{{\bf R}^k} \rho_k(\lambda_1,\ldots,\lambda_k) F(\lambda_1,\ldots,\lambda_k)\ d\lambda_1 \ldots d\lambda_k \ \ \ \ \ (22)$

$\displaystyle = \mathop{\bf E} \sum_{1 \leq i_1, \ldots, i_k \leq n, \hbox{ distinct}} F( \lambda_{i_1}(M_n),\ldots,\lambda_{i_k}(M_n) )$

for any test function ${F: {\bf R}^k \rightarrow {\bf C}}$ supported in the region ${\{ (x_1,\ldots,x_k): x_1 \leq \ldots \leq x_k \}}$.

In particular, if we set ${k=1}$, we obtain the explicit formula

$\displaystyle \mathop{\bf E} \mu_{M_n} = \frac{1}{n} K_n(x,x)\ dx$

for the expected empirical spectral measure of ${M_n}$. Equivalently after renormalising by ${\sqrt{n}}$, we have

$\displaystyle \mathop{\bf E} \mu_{M_n/\sqrt{n}} = \frac{1}{n^{1/2}} K_n(\sqrt{n}x,\sqrt{n}x)\ dx. \ \ \ \ \ (23)$

It is thus of interest to understand the kernel ${K_n}$ better.

To do this, we begin by recalling that the functions ${P_i(x) e^{-x^2/4}}$ were obtained from ${x^i e^{-x^2/4}}$ by the Gram-Schmidt process. In particular, each ${P_i(x) e^{-x^2/4}}$ is orthogonal to the ${x^j e^{-x^2/4}}$ for all ${0 \leq j. This implies that ${x P_i(x) e^{-x^2/4}}$ is orthogonal to ${x^j e^{-x^2/4}}$ for ${0 \leq j < i-1}$. On the other hand, ${xP_i(x)}$ is a polynomial of degree ${i+1}$, so ${x P_i(x) e^{-x^2/4}}$ must lie in the span of ${x^j e^{-x^2/4}}$ for ${0 \leq j \leq i+1}$. Combining the two facts, we see that ${x P_i}$ must be a linear combination of ${P_{i-1}, P_i, P_{i+1}}$, with the ${P_{i+1}}$ coefficient being non-trivial. We rewrite this fact in the form

$\displaystyle P_{i+1}(x) = (a_i x + b_i) P_i(x) - c_i P_{i-1}(x) \ \ \ \ \ (24)$

for some real numbers ${a_i,b_i,c_i}$ (with ${c_0=0}$). Taking inner products with ${P_{i+1}}$ and ${P_{i-1}}$ we see that

$\displaystyle \int_{\bf R} x P_i(x) P_{i+1}(x) e^{-x^2/2}\ dx = \frac{1}{a_i} \ \ \ \ \ (25)$

and

$\displaystyle \int_{\bf R} x P_i(x) P_{i-1}(x) e^{-x^2/2}\ dx = \frac{c_i}{a_i}$

and so

$\displaystyle c_i := \frac{a_i}{a_{i-1}} \ \ \ \ \ (26)$

(with the convention ${a_{-1}=\infty}$).

We will continue the computation of ${a_i,b_i,c_i}$ later. For now, we we pick two distinct real numbers ${x,y}$ and consider the Wronskian-type expression

$\displaystyle P_{i+1}(x) P_i(y) - P_i(x) P_{i+1}(y).$

Using (24), (26), we can write this as

$\displaystyle a_i(x-y) P_i(x) P_i(y) + \frac{a_i}{a_{i-1}} (P_{i-1}(x) P_i(y) - P_i(x) P_{i-1}(y))$

or in other words

$\displaystyle P_i(x) P_i(y) = \frac{P_{i+1}(x) P_i(y) - P_i(x) P_{i+1}(y)}{a_i(x-y)}$

$\displaystyle - \frac{P_i(x) P_{i-1}(y) - P_{i-1}(x) P_i(y)}{a_{i-1}(x-y)}.$

We telescope this and obtain the Christoffel-Darboux formula for the kernel (15):

$\displaystyle K_n(x,y) = \frac{P_{n}(x)P_{n-1}(y) - P_{n-1}(x) P_{n}(y)}{a_{n-1}(x-y)} e^{-(x^2+y^2)/4}. \ \ \ \ \ (27)$

Sending ${y \rightarrow x}$ using L’Hopital’s rule, we obtain in particular that

$\displaystyle K_n(x,x) = \frac{1}{a_{n-1}}( P'_{n}(x)P_{n-1}(x) - P'_{n-1}(x) P_{n}(x) ) e^{-x^2/2}. \ \ \ \ \ (28)$

Inserting this into (23), we see that if we want to understand the expected spectral measure of GUE, we should understand the asymptotic behaviour of ${P_n}$ and the associated constants ${a_n}$. For this, we need to exploit the specific properties of the gaussian weight ${e^{-x^2/2}}$. In particular, we have the identity

$\displaystyle x e^{-x^2/2} = - \frac{d}{dx} e^{-x^2/2} \ \ \ \ \ (29)$

so upon integrating (25) by parts, we have

$\displaystyle \int_{\bf R} (P'_i(x) P_{i+1}(x) + P_i(x) P'_{i+1}(x)) e^{-x^2/2}\ dx = \frac{1}{a_i}.$

As ${P'_i}$ has degree at most ${i-1}$, the first term vanishes by the orthonormal nature of the ${P_i(x) e^{-x^2/4}}$, thus

$\displaystyle \int_{\bf R} P_i(x) P'_{i+1}(x) e^{-x^2/2}\ dx = \frac{1}{a_i}. \ \ \ \ \ (30)$

To compute this, let us denote the leading coefficient of ${P_i}$ as ${k_i}$. Then ${P'_{i+1}}$ is equal to ${\frac{(i+1)k_{i+1}}{k_i} P_i}$ plus lower-order terms, and so we have

$\displaystyle \frac{(i+1)k_{i+1}}{k_i} = \frac{1}{a_i}.$

On the other hand, by inspecting the ${x^{i+1}}$ coefficient of (24) we have

$\displaystyle k_{i+1} = a_i k_i.$

Combining the two formulae (and making the sign convention that the ${k_i}$ are always positive), we see that

$\displaystyle a_i = \frac{1}{\sqrt{i+1}}$

and

$\displaystyle k_{i+1} = \frac{k_i}{\sqrt{i+1}}.$

Meanwhile, a direct computation shows that ${P_0(x) = k_0 = \frac{1}{(2\pi)^{1/4}}}$, and thus by induction

$\displaystyle k_i := \frac{1}{(2\pi)^{1/4} \sqrt{i!}}.$

A similar method lets us compute the ${b_i}$. Indeed, taking inner products of (24) with ${P_i(x) e^{-x^2/2}}$ and using orthonormality we have

$\displaystyle b_i = - a_i \int_{\bf R} x P_i(x)^2 e^{-x^2/2}\ dx$

which upon integrating by parts using (29) gives

$\displaystyle b_i = - 2 a_i \int_{\bf R} P_i(x) P'_i(x) e^{-x^2/2}\ dx.$

As ${P'_i}$ is of degree strictly less than ${i}$, the integral vanishes by orthonormality, thus ${b_i=0}$. The identity (24) thus becomes Hermite recurrence relation

$\displaystyle P_{i+1}(x) = \frac{1}{\sqrt{i+1}} x P_i(x) - \frac{\sqrt{i}}{\sqrt{i+1}} P_{i-1}(x). \ \ \ \ \ (31)$

Another recurrence relation arises by considering the integral

$\displaystyle \int_{\bf R} P_j(x) P'_{i+1}(x) e^{-x^2/2}\ dx.$

On the one hand, as ${P'_{i+1}}$ has degree at most ${i}$, this integral vanishes if ${j>i}$ by orthonormality. On the other hand, integrating by parts using (29), we can write the integral as

$\displaystyle \int_{\bf R} (xP_j - P'_j)(x) P_{i+1}(x) e^{-x^2/2}\ dx.$

If ${j < i}$, then ${xP_j-P'_j}$ has degree less than ${i+1}$, so the integral again vanishes. Thus the integral is non-vanishing only when ${j=i}$. Using (30), we conclude that

$\displaystyle P'_{i+1} = \frac{1}{a_i} P_i = \sqrt{i+1} P_i. \ \ \ \ \ (32)$

We can combine (32) with (31) to obtain the formula

$\displaystyle \frac{d}{dx}( e^{-x^2/2} P_i(x) ) = - \sqrt{i+1} e^{-x^2/2} P_{i+1}(x),$

which together with the initial condition ${P_0 = \frac{1}{(2\pi)^{1/4}}}$ gives the explicit representation

$\displaystyle P_n(x) := \frac{(-1)^n}{(2\pi)^{1/4} \sqrt{n!}} e^{x^2/2} \frac{d^n}{dx^n} e^{-x^2/2} \ \ \ \ \ (33)$

for the Hermite polynomials. Thus, for instance, at ${x=0}$ one sees from Taylor expansion that

$\displaystyle P_n(0) = \frac{(-1)^{n/2}\sqrt{n!}}{(2\pi)^{1/4} 2^{n/2} (n/2)!} ;\quad P'_n(0) = 0 \ \ \ \ \ (34)$

when ${n}$ is even, and

$\displaystyle P_n(0) = 0;\quad P'_n(0) = \frac{(-1)^{(n+1)/2} (n+1) \sqrt{n!}}{(2\pi)^{1/4} 2^{(n+1)/2} ((n+1)/2)!} \ \ \ \ \ (35)$

when ${n}$ is odd.

In principle, the formula (33), together with (28), gives us an explicit description of the kernel ${K_n(x,x)}$ (and thus of ${\mathop{\bf E} \mu_{M_n/\sqrt{n}}}$, by (23)). However, to understand the asymptotic behaviour as ${n \rightarrow \infty}$, we would have to understand the asymptotic behaviour of ${\frac{d^n}{dx^n} e^{-x^2/2}}$ as ${n \rightarrow \infty}$, which is not immediately discernable by inspection. However, one can obtain such asymptotics by a variety of means. We give two such methods here: a method based on ODE analysis, and a complex-analytic method, based on the method of steepest descent.

We begin with the ODE method. Combining (31) with (32) we see that each polynomial ${P_m}$ obeys the Hermite differential equation

$\displaystyle P''_m(x) - x P'_m(x) + m P_m(x) = 0.$

If we look instead at the Hermite functions ${\phi_m(x) := P_m(x) e^{-x^2/4}}$, we obtain the differential equation

$\displaystyle L \phi_m(x) = (m+\frac{1}{2}) \phi_m$

where ${L}$ is the harmonic oscillator operator

$\displaystyle L \phi := - \phi'' + \frac{x^2}{4} \phi.$

Note that the self-adjointness of ${L}$ here is consistent with the orthogonal nature of the ${\phi_m}$.

Exercise 5 Use (15), (28), (33), (31), (32) to establish the identities

$\displaystyle K_n(x,x) = \sum_{j=0}^{n-1} \phi_j(x)^2$

$\displaystyle = \phi'_n(x)^2 + (n - \frac{x^2}{4}) \phi_n(x)^2$

and thus by (23)

$\displaystyle \mathop{\bf E} \mu_{M_n/\sqrt{n}} = \frac{1}{\sqrt{n}} \sum_{j=0}^{n-1} \phi_j(\sqrt{n} x)^2\ dx =$

$\displaystyle = [\frac{1}{\sqrt{n}} \phi'_n(\sqrt{n} x)^2 + \sqrt{n} (1 - \frac{x^2}{4}) \phi_n(\sqrt{n} x)^2]\ dx.$

It is thus natural to look at the rescaled functions

$\displaystyle \tilde \phi_m(x) := \sqrt{n} \phi_m(\sqrt{n} x)$

which are orthonormal in ${L^2({\bf R})}$ and solve the equation

$\displaystyle L_{1/n} \tilde \phi_m(x) = \frac{m+1/2}{n} \tilde \phi_m$

where ${L_h}$ is the semiclassical harmonic oscillator operator

$\displaystyle L_h \phi := - h^2 \phi'' + \frac{x^2}{4} \phi,$

thus

$\displaystyle \mathop{\bf E} \mu_{M_n/\sqrt{n}} = \frac{1}{n} \sum_{j=0}^{n-1} \tilde \phi_j(x)^2\ dx =$

$\displaystyle = [\frac{1}{n} \tilde \phi'_n(x)^2 + (1 - \frac{x^2}{4}) \tilde \phi_n(x)^2]\ dx. \ \ \ \ \ (36)$

The projection ${\pi_{V_n}}$ is then the spectral projection operator of ${L_{1/\sqrt{n}}}$ to ${[0,1]}$. According to semi-classical analysis, with ${h}$ being interpreted as analogous to Planck’s constant, the operator ${L_h}$ has symbol ${p^2 + \frac{x^2}{4}}$, where ${p := -i h \frac{d}{dx}}$ is the momentum operator, so the projection ${\pi_{V_n}}$ is a projection to the region ${\{ (x,p): p^2 + \frac{x^2}{4} \leq 1 \}}$ of phase space, or equivalently to the region ${\{ (x,p): |p| < (4-x^2)_+^{1/2}\}}$. In the semi-classical limit ${h \rightarrow 0}$, we thus expect the diagonal ${K_n(x,x)}$ of the normalised projection ${h^2 \pi_{V_n}}$ to be proportional to the projection of this region to the ${x}$ variable, i.e. proportional to ${(4-x^2)_+^{1/2}}$. We are thus led to the semi-circular law via semi-classical analysis.

It is possible to make the above argument rigorous, but this would require developing the theory of microlocal analysis, which would be overkill given that we are just dealing with an ODE rather than a PDE here (and an extremely classical ODE at that). We instead use a more basic semiclassical approximation, the WKB approximation, which we will make rigorous using the classical method of variation of parameters (one could also proceed using the closely related Prüfer transformation, which we will not detail here). We study the eigenfunction equation

$\displaystyle L_h \phi = \lambda \phi$

where we think of ${h > 0}$ as being small, and ${\lambda}$ as being close to ${1}$. We rewrite this as

$\displaystyle \phi'' = - \frac{1}{h^2} k(x)^2 \phi \ \ \ \ \ (37)$

where ${k(x) := \sqrt{\lambda - x^2/4}}$, where we will only work in the “classical” region ${x^2/4 < \lambda}$ (so ${k(x) > 0}$) for now.

Recall that the general solution to the constant coefficient ODE ${\phi'' = -\frac{1}{h^2} k^2 \phi}$ is given by ${\phi(x) = A e^{ikx/h} + B e^{-ikx/h}}$. Inspired by this, we make the ansatz

$\displaystyle \phi(x) = A(x) e^{i \Psi(x)/h} + B(x) e^{-i \Psi(x)/h}$

where ${\Psi(x) := \int_0^x k(y)\ dy}$ is the antiderivative of ${k}$. Differentiating this, we have

$\displaystyle \phi'(x) = \frac{i k(x)}{h}( A(x) e^{i\Psi(x)/h} - B(x) e^{-i\Psi(x)/h} )$

$\displaystyle + A'(x) e^{i\Psi(x)/h} + B'(x) e^{-i\Psi(x)/h}.$

Because we are representing a single function ${\phi}$ by two functions ${A, B}$, we have the freedom to place an additional constraint on ${A,B}$. Following the usual variation of parameters strategy, we will use this freedom to eliminate the last two terms in the expansion of ${\phi}$, thus

$\displaystyle A'(x) e^{i\Psi(x)/h} + B'(x) e^{-i\Psi(x)/h} = 0. \ \ \ \ \ (38)$

We can now differentiate again and obtain

$\displaystyle \phi''(x) = -\frac{k(x)^2}{h^2} \phi(x) + \frac{ik'(x)}{h} ( A(x) e^{i\Psi(x)/h} - B(x) e^{-i\Psi(x)/h} )$

$\displaystyle + \frac{ik(x)}{h} ( A'(x) e^{i\Psi(x)/h} - B'(x) e^{-i\Psi(x)/h} ).$

Comparing this with (37) we see that

$\displaystyle A'(x) e^{i\Psi(x)/h} - B'(x) e^{-i\Psi(x)/h} = - \frac{k'(x)}{k(x)} ( A(x) e^{i\Psi(x)/h} - B(x) e^{-i\Psi(x)/h} ).$

Combining this with (38), we obtain equations of motion for ${A}$ and ${B}$:

$\displaystyle A'(x) = - \frac{k'(x)}{2 k(x)} A(x) + \frac{k'(x)}{2 k(x)} B(x) e^{-2i\Psi(x)/h}$

$\displaystyle B'(x) = - \frac{k'(x)}{2 k(x)} B(x) + \frac{k'(x)}{2 k(x)} A(x) e^{2i\Psi(x)/h}.$

We can simplify this using the integrating factor substitution

$\displaystyle A(x) = k(x)^{-1/2} a(x); \quad B(x) = k(x)^{-1/2} b(x)$

to obtain

$\displaystyle a'(x) = \frac{k'(x)}{2 k(x)} b(x) e^{-2i\Psi(x)/h}; \ \ \ \ \ (39)$

$\displaystyle b'(x) = \frac{k'(x)}{2 k(x)} a(x) e^{2i\Psi(x)/h}. \ \ \ \ \ (40)$

The point of doing all these transformations is that the role of the ${h}$ parameter no longer manifests itself through amplitude factors, and instead only is present in a phase factor. In particular, we have

$\displaystyle a', b' = O( |a| + |b| )$

on any compact interval ${I}$ in the interior of the classical region ${x^2/4 < \lambda}$ (where we allow implied constants to depend on ${I}$), which by Gronwall’s inequality gives the bounds

$\displaystyle a'(x), b'(x), a(x), b(x) = O( |a(0)| + |b(0)| )$

on this interval ${I}$. We can then insert these bounds into (39), (40) again and integrate by parts (taking advantage of the non-stationary nature of ${\Psi}$) to obtain the improved bounds

$\displaystyle a(x) = a(0) + O( h (|a(0)|+|b(0)|) ); \quad b(x) = b(0) + O(h (|a(0)|+|b(0)|) ) \ \ \ \ \ (41)$

on this interval. (More precise asymptotic expansions can be obtained by iterating this procedure, but we will not need them here.) This is already enough to get the asymptotics that we need:

Exercise 6 Use (36) to Show that on any compact interval ${I}$ in ${(-2,2)}$, the density of ${\mathop{\bf E} \mu_{M_n/\sqrt{n}}}$ is given by

$\displaystyle (|a|^2(x)+|b|^2(x)) ( \sqrt{1-x^2/4} + o(1) ) + O( |a(x)| |b(x)| )$

where ${a, b}$ are as above with ${\lambda=1+\frac{1}{2n}}$ and ${h=\frac{1}{n}}$. Combining this with (41), (34), (35), and Stirling’s formula, conclude that ${\mathop{\bf E} \mu_{M_n/\sqrt{n}}}$ converges in the vague topology to the semicircular law ${\frac{1}{2\pi} (4-x^2)_+^{1/2}\ dx}$. (Note that once one gets convergence inside ${(-2,2)}$, the convergence outside of ${[-2,2]}$ can be obtained for free since ${\mu_{M_n/\sqrt{n}}}$ and ${\frac{1}{2\pi} (4-x^2)_+^{1/2}\ dx}$ are both probability measures.

We now sketch out the approach using the method of steepest descent. The starting point is the Fourier inversion formula

$\displaystyle e^{-x^2/2} = \frac{1}{\sqrt{2\pi}} \int_{\bf R} e^{itx} e^{-t^2/2}\ dt$

which upon repeated differentiation gives

$\displaystyle \frac{d^n}{dx^n} e^{-x^2/2} = \frac{i^n}{\sqrt{2\pi}} \int_{\bf R} t^n e^{itx} e^{-t^2/2}\ dt$

and thus by (33)

$\displaystyle P_n(x) = \frac{(-i)^n}{(2\pi)^{3/4} \sqrt{n!}} \int_{\bf R} t^n e^{-(t-ix)^2/2}\ dt$

and thus

$\displaystyle \tilde \phi_n(x) = \frac{(-i)^n}{(2\pi)^{3/4} \sqrt{n!}} n^{(n+1)/2} \int_{\bf R} e^{n \phi(t)} \ dt$

where

$\displaystyle \phi(t) := \log t - (t-ix)^2/2 - x^2/4$

where we use a suitable branch of the complex logarithm to handle the case of negative ${t}$.

The idea of the principle of steepest descent is to shift the contour of integration to where the real part of ${\phi(z)}$ is as small as possible. For this, it turns out that the stationary points of ${\phi(z)}$ play a crucial role. A brief calculation using the quadratic formula shows that there are two such stationary points, at

$\displaystyle z = \frac{ix \pm \sqrt{4-x^2}}{2}.$

When ${|x| < 2}$, ${\phi}$ is purely imaginary at these stationary points, while for ${|x| > 2}$ the real part of ${\phi}$ is negative at both points. One then draws a contour through these two stationary points in such a way that near each such point, the imaginary part of ${\phi(z)}$ is kept fixed, which keeps oscillation to a minimum and allows the real part to decay as steeply as possible (which explains the name of the method). After a certain tedious amount of computation, one obtains the same type of asymptotics for ${\tilde \phi_n}$ that were obtained by the ODE method when ${|x| < 2}$ (and exponentially decaying estimates for ${|x|>2}$).

Exercise 7 Let ${f: {\bf C} \rightarrow {\bf C}}$, ${g:{\bf C} \rightarrow {\bf C}}$ be functions which are analytic near a complex number ${z_0}$, with ${f'(z_0) = 0}$ and ${f''(z_0) \neq 0}$. Let ${\epsilon > 0}$ be a small number, and let ${\gamma}$ be the line segment ${\{ z_0 + t v: -\epsilon < t < \epsilon \}}$, where ${v}$ is a complex phase such that ${f''(z_0) v^2}$ is a negative real. Show that for ${\epsilon}$ sufficiently small, one has

$\displaystyle \int_\gamma e^{\lambda f(z)} g(z)\ dz = (1+o(1)) \frac{\sqrt{2\pi} v}{\sqrt{f''(z_0) \lambda}} e^{\lambda f(z_0)} g(z_0)$

as ${\lambda \rightarrow +\infty}$. This is the basic estimate behind the method of steepest descent; readers who are also familiar with the method of stationary phase may see a close parallel.

Remark 6 The method of steepest descent requires an explicit representation of the orthogonal polynomials as contour integrals, and as such is largely restricted to the classical orthogonal polynomials (such as the Hermite polynomials). However, there is a non-linear generalisation of the method of steepest descent developed by Deift and Zhou, in which one solves a matrix Riemann-Hilbert problem rather than a contour integral; see this book by Deift for details. Using these sorts of tools, one can generalise much of the above theory to the spectral distribution of ${U(n)}$-conjugation-invariant discussed in Remark 2, with the theory of Hermite polynomials being replaced by the more general theory of orthogonal polynomials; this is discussed in the above book of Deift, as well as the more recent book of Deift and Gioev.

The computations performed above for the diagonal kernel ${K_n(x,x)}$ can be summarised by the asymptotic

$\displaystyle K_n( \sqrt{n} x, \sqrt{n} x ) = \sqrt{n} ( \rho_{sc}(x) + o(1) )$

whenever ${x \in {\bf R}}$ is fixed and ${n \rightarrow \infty}$, and ${\rho_{sc}(x) := \frac{1}{2\pi} (4-x^2)_+^{1/2}}$ is the semi-circular law distribution. It is reasonably straightforward to generalise these asymptotics to the off-diagonal case as well, obtaining the more general result

$\displaystyle K_n( \sqrt{n} x + \frac{y_1}{\sqrt{n} \rho_{sc}(x)}, \sqrt{n} x + \frac{y_2}{\sqrt{n} \rho_{sc}(x)} ) = \sqrt{n} ( \rho_{sc}(x) K(y_1,y_2) + o(1) ) \ \ \ \ \ (42)$

for fixed ${x \in (-2,2)}$ and ${y_1,y_2 \in {\bf R}}$, where ${K}$ is the Dyson sine kernel

$\displaystyle K(y_1,y_2) := \frac{\sin(\pi(y_1-y_2)}{\pi(y_1-y_2)}.$

In the language of semi-classical analysis, what is going on here is that the rescaling in the left-hand side of (42) is transforming the phase space region ${\{ (x,p): p^2 + \frac{x^2}{4} \leq 1 \}}$ to the region ${\{ (x,p): |p| \leq 1 \}}$ in the limit ${n \rightarrow \infty}$, and the projection to the latter region is given by the Dyson sine kernel. A formal proof of (42) can be given by using either the ODE method or the steepest descent method to obtain asymptotics for Hermite polynomials, and thence (via the Christoffel-Darboux formula) to asymptotics for ${K_n}$; we do not give the details here, but see for instance the recent book of Anderson, Guionnet, and Zeitouni.

From (42) and (21), (22) we obtain the asymptotic formula

$\displaystyle \mathop{\bf E} \sum_{1 \leq i_1 < \ldots < i_k \leq n} F( \sqrt{n} \rho_{sc}(x) (\lambda_{i_1}(M_n) - \sqrt{n} x),\ldots,$

$\displaystyle \sqrt{n} \rho_{sc}(x) (\lambda_{i_k}(M_n) - \sqrt{n} x) )$

$\displaystyle \rightarrow \int_{{\bf R}^k} F(y_1,\ldots,y_k) \det(K(y_i,y_j))_{1 \leq i,j \leq k}\ dy_1 \ldots dy_k$

for the local statistics of eigenvalues. By means of further algebraic manipulations (using the general theory of determinantal processes), this allows one to control such quantities as the distribution of eigenvalue gaps near ${\sqrt{n} x}$, normalised at the scale ${\frac{1}{\sqrt{n} \rho_{sc}(x)}}$, which is the average size of these gaps as predicted by the semicircular law. For instance, for any ${s_0>0}$, one can show (basically by the above formulae combined with the inclusion-exclusion principle) that the proportion of eigenvalues ${\lambda_i}$ with normalised gap ${\sqrt{n} \frac{\lambda_{i+1}-\lambda_i}{\rho_{sc}(t_{i/n})}}$ less than ${s_0}$ converges as ${n \rightarrow \infty}$ to ${\int_0^{s_0} \frac{d^2}{ds^2} \det(1-K)_{L^2[0,s]}\ ds}$, where ${t_c \in [-2,2]}$ is defined by the formula ${\int_{-2}^{t_c} \rho_{sc}(x)\ dx = c}$, and ${K}$ is the integral operator with kernel ${K(x,y)}$ (this operator can be verified to be trace class, so the determinant can be defined in a Fredholm sense). See for instance this book of Mehta (and my blog post on determinantal processes describe a finitary version of the inclusion-exclusion argument used to obtain such a result).

Remark 7 One can also analyse the distribution of the eigenvalues at the edge of the spectrum, i.e. close to ${\pm 2 \sqrt{n}}$. This ultimately hinges on understanding the behaviour of the projection ${\pi_{V_n}}$ near the corners ${(0, \pm 2)}$ of the phase space region ${\Omega = \{ (p,x): p^2 + \frac{x^2}{4} \leq 1 \}}$, or of the Hermite polynomials ${P_n(x)}$ for ${x}$ close to ${\pm 2 \sqrt{n}}$. For instance, by using steepest descent methods, one can show that

$\displaystyle n^{1/12} \phi_n(2\sqrt{n} + n^{1/6} x) \rightarrow Ai(x)$

as ${n \rightarrow \infty}$ for any fixed ${x,y}$, where ${Ai}$ is the Airy function

$\displaystyle Ai(x) := \frac{1}{\pi} \int_0^\infty \cos( \frac{t^3}{3} + tx )\ dt.$

This asymptotic and the Christoffel-Darboux formula then gives the asymptotic

$\displaystyle n^{1/6} K_n(2\sqrt{n} + n^{1/6} x, 2\sqrt{n} + n^{1/6} y) \rightarrow K_{Ai}(x,y) \ \ \ \ \ (43)$

for any fixed ${x,y}$, where ${K_{Ai}}$ is the Airy kernel

$\displaystyle K_{Ai}(x,y) := \frac{Ai(x) Ai'(y) - Ai'(x) Ai(y)}{x-y}.$

(Aside: Semiclassical heuristics suggest that the rescaled kernel (43) should correspond to projection to the parabolic region of phase space ${\{ (p,x): p^2 + x \leq 1\}}$, but I do not know of a connection between this region and the Airy kernel; I am not sure whether semiclassical heuristics are in fact valid at this scaling regime. On the other hand, these heuristics do explain the emergence of the length scale ${n^{1/6}}$ that emerges in (43), as this is the smallest scale at the edge which occupies a region in ${\Omega}$ consistent with the Heisenberg uncertainty principle.) This then gives an asymptotic description of the largest eigenvalues of a GUE matrix, which cluster in the region ${2\sqrt{n} + O(n^{1/6})}$. For instance, one can use the above asymptotics to show that the largest eigenvalue ${\lambda_1}$ of a GUE matrix obeys the Tracy-Widom law

$\displaystyle \mathop{\bf P}( \frac{\lambda_1 - 2\sqrt{n}}{n^{1/6}} < t ) \rightarrow \det(1 - A)_{L^2[0,t]}$

for any fixed ${t}$, where ${A}$ is the integral operator with kernel ${K_{Ai}}$. See for instance the recent book of Anderson, Guionnet, and Zeitouni.

— 5. Determinantal form of the gaussian matrix distribution —

One can perform an analogous analysis of the joint distribution function (10) of gaussian random matrices. Indeed, given any family ${P_0,\ldots,P_{n-1}(z)}$ of polynomials, with each ${P_i}$ of degree ${i}$, much the same arguments as before show that (10) is equal to a constant multiple of

$\displaystyle \det( \sum_{k=0}^{n-1} P_k(\lambda_i) e^{-|\lambda_i|^2/2} \overline{P_k(\lambda_j)} e^{-|\lambda_j|^2/2} )_{1 \leq i,j \leq n}.$

One can then select ${P_k(z) e^{-|z|^2/2}}$ to be orthonormal in ${L^2({\bf C})}$. Actually in this case, the polynomials are very simple, being given explicitly by the formula

$\displaystyle P_k(z) := \frac{1}{\sqrt{\pi k!}} z^k.$

Exercise 8 Verify that the ${P_k(z) e^{-|z|^2/2}}$ are indeed orthonormal, and then conclude that (10) is equal to ${\det( K_n(\lambda_i,\lambda_j) )_{1 \leq i,j \leq n}}$, where

$\displaystyle K_n(z,w) := \frac{1}{\pi} e^{-(|z|^2+|w|^2)/2} \sum_{k=0}^{n-1} \frac{(z\overline{w})^k}{k!}.$

Conclude further that the ${m}$-point correlation functions ${\rho_m(z_1,\ldots,z_m)}$ are given as

$\displaystyle \rho_m(z_1,\ldots,z_m) = \det( K_n(z_i,z_j) )_{1 \leq i,j \leq m}.$

Exercise 9 Show that as ${n \rightarrow \infty}$, one has

$\displaystyle K_n( \sqrt{n} z, \sqrt{n} z ) = \frac{1}{\pi} 1_{|z| \leq 1} + o(1)$

and deduce that the expected spectral measure ${{\bf E} \mu_{G/\sqrt{n}}}$ converges vaguely to the circular measure ${\mu_c := \frac{1}{\pi} 1_{|z| \leq 1}\ dz}$; this is a special case of the circular law.

Exercise 10 For any ${|z| < 1}$ and ${w_1, w_2 \in {\bf C}}$, show that

$\displaystyle K_n( \sqrt{n} (z+w_1), \sqrt{n} (z+w_2) ) = \frac{1}{\pi} \exp( - |w_1-w_2|^2 / 2 ) + o(1)$

as ${n \rightarrow \infty}$. This formula (in principle, at least) describes the asymptotic local ${m}$-point correlation functions of the spectrum of gaussian matrices.

Remark 8 One can use the above formulae as the starting point for many other computations on the spectrum of random gaussian matrices; to give just one example, one can show that expected number of eigenvalues which are real is of the order of ${\sqrt{n}}$ (see this paper of Edelman for more precise results of this nature). It remains a challenge to extend these results to more general ensembles than the gaussian ensemble.