Lieb–Thirring inequality

For the Schrödinger operator ${\displaystyle -\Delta +V(x)=-\nabla ^{2}+V(x)}$ on ${\displaystyle \mathbb {R} ^{n}}$ with real-valued potential ${\displaystyle V(x):\mathbb {R} ^{n}\to \mathbb {R} ,}$ the numbers ${\displaystyle \lambda _{1}\leq \lambda _{2}\leq \dots \leq 0}$ denote the (not necessarily finite) sequence of negative eigenvalues. Then, for ${\displaystyle \gamma }$ and ${\displaystyle n}$ satisfying one of the conditions

${\displaystyle {\begin{aligned}\gamma \geq {\frac {1}{2}}&,\,n=1,\\\gamma >0&,\,n=2,\\\gamma \geq 0&,\,n\geq 3,\end{aligned}}}$

there exists a constant ${\displaystyle L_{\gamma ,n}}$, which only depends on ${\displaystyle \gamma }$ and ${\displaystyle n}$, such that

${\displaystyle \sum _{j\geq 1}|\lambda _{j}|^{\gamma }\leq L_{\gamma ,n}\int _{\mathbb {R} ^{n}}V(x)_{-}^{\gamma +{\frac {n}{2}}}\mathrm {d} ^{n}x}$

(1)

where ${\displaystyle V(x)_{-}:=\max(-V(x),0)}$ is the negative part of the potential ${\displaystyle V}$. The cases ${\displaystyle \gamma >1/2,n=1}$ as well as ${\displaystyle \gamma >0,n\geq 2}$ were proven by E. H. Lieb and W. E. Thirring in 1976 [1] and used in their proof of stability of matter. In the case ${\displaystyle \gamma =0,n\geq 3}$ the left-hand side is simply the number of negative eigenvalues, and proofs were given independently by M. Cwikel,[2] E. H. Lieb [3] and G. V. Rozenbljum.[4] The resulting ${\displaystyle \gamma =0}$ inequality is thus also called the Cwikel–Lieb–Rosenbljum bound. The remaining critical case ${\displaystyle \gamma =1/2,n=1}$ was proven to hold by T. Weidl [5] The conditions on ${\displaystyle \gamma }$ and ${\displaystyle n}$ are necessary and cannot be relaxed.

The Lieb–Thirring inequality for ${\displaystyle \gamma =1}$ is equivalent to a lower bound on the kinetic energy of a given normalised ${\displaystyle N}$-particle wave function ${\displaystyle \psi \in L^{2}(\mathbb {R} ^{Nn})}$ in terms of the one-body density. For an anti-symmetric wave function such that

${\displaystyle \psi (x_{1},\dots ,x_{i},\dots ,x_{j},\dots ,x_{N})=-\psi (x_{1},\dots ,x_{j},\dots ,x_{i},\dots ,x_{N})}$

for all ${\displaystyle 1\leq i,j\leq N}$, the one-body density is defined as

${\displaystyle \rho _{\psi }(x)=N\int _{\mathbb {R} ^{(N-1)n}}|\psi (x,x_{2}\dots ,x_{N})|^{2}\mathrm {d} ^{n}x_{2}\cdots \mathrm {d} ^{n}x_{N},\,x\in \mathbb {R} ^{n}.}$

The Lieb–Thirring inequality (1) for ${\displaystyle \gamma =1}$ is equivalent to the statement that

${\displaystyle \sum _{i=1}^{N}\int _{\mathbb {R} ^{n}}|\nabla _{i}\psi |^{2}\mathrm {d} ^{n}x_{i}\geq K_{n}\int _{\mathbb {R} ^{n}}{\rho _{\psi }(x)^{1+{\frac {2}{n}}}}\mathrm {d} ^{n}x}$

(2)

where the sharp constant ${\displaystyle K_{n}}$ is defined via

${\displaystyle \left(\left(1+{\frac {2}{n}}\right)K_{n}\right)^{1+{\frac {n}{2}}}\left(\left(1+{\frac {n}{2}}\right)L_{1,n}\right)^{1+{\frac {2}{n}}}=1\,.}$

The inequality can be extended to particles with spin states by replacing the one-body density by the spin-summed one-body density. The constant ${\displaystyle K_{n}}$ then has to be replaced by ${\displaystyle K_{n}/q^{2/n}}$ where ${\displaystyle q}$ is the number of quantum spin states available to each particle (${\displaystyle q=2}$ for electrons). If the wave function is symmetric, instead of anti-symmetric, such that

${\displaystyle \psi (x_{1},\dots ,x_{i},\dots ,x_{j},\dots ,x_{n})=\psi (x_{1},\dots ,x_{j},\dots ,x_{i},\dots ,x_{n})}$

for all ${\displaystyle 1\leq i,j\leq N}$, the constant ${\displaystyle K_{n}}$ has to be replaced by ${\displaystyle K_{n}/N^{2/n}}$. Inequality (2) describes the minimum kinetic energy necessary to achieve a given density ${\displaystyle \rho _{\psi }}$ with ${\displaystyle N}$ particles in ${\displaystyle n}$ dimensions. If ${\displaystyle L_{1,3}=L_{1,3}^{\mathrm {cl} }}$ was proven to hold, the right-hand side of (2) for ${\displaystyle n=3}$ would be precisely the kinetic energy term in Thomas–Fermi theory.

The inequality can be compared to the Sobolev inequality. M. Rumin[12] derived the kinetic energy inequality (2) (with a smaller constant) directly without the use of the Lieb–Thirring inequality.

(for more information, read the Stability of matter page)

The kinetic energy inequality plays an important role in the proof of stability of matter as presented by Lieb and Thirring.[1] The Hamiltonian under consideration describes a system of ${\displaystyle N}$ particles with ${\displaystyle q}$ spin states and ${\displaystyle M}$ fixed nuclei at locations ${\displaystyle R_{j}\in \mathbb {R} ^{3}}$ with charges ${\displaystyle Z_{j}>0}$. The particles and nuclei interact with each other through the electrostatic Coulomb force and an arbitrary magnetic field can be introduced. If the particles under consideration are fermions (i.e. the wave function ${\displaystyle \psi }$ is antisymmetric), then the kinetic energy inequality (2) holds with the constant ${\displaystyle K_{n}/q^{2/n}}$ (not ${\displaystyle K_{n}/N^{2/n}}$). This is a crucial ingredient in the proof of stability of matter for a system of fermions. It ensures that the ground state energy ${\displaystyle E_{N,M}(Z_{1},\dots ,Z_{M})}$ of the system can be bounded from below by a constant depending only on the maximum of the nuclei charges, ${\displaystyle Z_{\max }}$, times the number of particles,

${\displaystyle E_{N,M}(Z_{1},\dots ,Z_{M})\geq -C(Z_{\max })(M+N)\,.}$

The system is then stable of the first kind since the ground-state energy is bounded from below and also stable of the second kind, i.e. the energy of decreases linearly with the number of particles and nuclei. In comparison, if the particles are assumed to be bosons (i.e. the wave function ${\displaystyle \psi }$ is symmetric), then the kinetic energy inequality (2) holds only with the constant ${\displaystyle K_{n}/N^{2/n}}$ and for the ground state energy only a bound of the form ${\displaystyle -CN^{5/3}}$ holds. Since the power ${\displaystyle 5/3}$ can be shown to be optimal, a system of bosons is stable of the first kind but unstable of the second kind.

If the Laplacian ${\displaystyle -\Delta =-\nabla ^{2}}$ is replaced by ${\displaystyle (\mathrm {i} \nabla +A(x))^{2}}$, where ${\displaystyle A(x)}$ is a magnetic field vector potential in ${\displaystyle \mathbb {R} ^{n},}$ the Lieb–Thirring inequality (1) remains true. The proof of this statement uses the diamagnetic inequality. Although all presently known constants ${\displaystyle L_{\gamma ,n}}$ remain unchanged, it is not known whether this is true in general for the best possible constant.

The Laplacian can also be replaced by other powers of ${\displaystyle -\Delta }$. In particular for the operator ${\displaystyle {\sqrt {-\Delta }}}$, a Lieb–Thirring inequality similar to (1) holds with a different constant ${\displaystyle L_{\gamma ,n}}$ and with the power on the right-hand side replaced by ${\displaystyle \gamma +n}$. Analogously a kinetic inequality similar to (2) holds, with ${\displaystyle 1+2/n}$ replaced by ${\displaystyle 1+1/n}$, which can be used to prove stability of matter for the relativistic Schrödinger operator under additional assumptions on the charges ${\displaystyle Z_{k}}$.[13]

In essence, the Lieb–Thirring inequality (1) gives an upper bound on the distances of the eigenvalues ${\displaystyle \lambda _{j}}$ to the essential spectrum ${\displaystyle [0,\infty )}$ in terms of the perturbation ${\displaystyle V}$. Similar inequalities can be proved for Jacobi operators.[14]

• Lieb, E.H.; Seiringer, R. (2010). The stability of matter in quantum mechanics (1st ed.). Cambridge: Cambridge University Press. ISBN 9780521191180.
• Hundertmark, D. (2007). "Some bound state problems in quantum mechanics". In Fritz Gesztesy; Percy Deift; Cherie Galvez; Peter Perry; Wilhelm Schlag (eds.). Spectral Theory and Mathematical Physics: A Festschrift in Honor of Barry Simon's 60th Birthday. Proceedings of Symposia in Pure Mathematics. Vol. 76. Providence, RI: American Mathematical Society. pp. 463–496. Bibcode:2007stmp.conf..463H. ISBN 978-0-8218-3783-2.