Mixing transformations in quantum field theory are nontrivial, since they are intimately related to the unitary inequivalence between Fock spaces for fields with definite mass and fields with definite flavor. Considering the superposition of two neutral scalar (spin-0) bosonic fields, we investigate some features of the emerging condensate structure of the flavor vacuum. In particular, we quantify the flavor vacuum entanglement in terms of the von Neumann entanglement entropy of the reduced state. Furthermore, in a suitable limit, we show that the flavor vacuum has a structure akin to the thermal vacuum of thermo field dynamics, with a temperature dependent on both the mixing angle and the particle mass difference.Mixing transformations in quantum field theory are nontrivial, since they are intimately related to the unitary inequivalence between Fock spaces for fields with definite mass and fields with definite flavor. Considering the superposition of two neutral scalar (spin-0) bosonic fields, we investigate some features of the emerging condensate structure of the flavor vacuum. In particular, we quantify the flavor vacuum entanglement in terms of the von Neumann entanglement entropy of the reduced state. Furthermore, in a suitable limit, we show that the flavor vacuum has a structure akin to the thermal vacuum of thermo field dynamics, with a temperature dependent on both the mixing angle and the particle mass difference.

arXiv:2101.04146Physical Review AMar 26, 202110 citations

Quantum Entanglement and Nonlocality

J. G. Cramer

Springer eBooksDec 23, 20155 citations

Uncountably many inequivalent maximally entangled measurements for two qutrits

Elna Svegborn, Jef Pauwels, Nicolas Gisin +1 more

Every two-qubit measurement basis composed of maximally entangled eigenstates can be transformed into the Bell basis via local unitary operations. For higher dimensions, in contrast, there exist inequivalent bases composed of maximally entangled eigenstates. Here, we provide a single-parameter family of two-qutrit maximally entangled measurement bases, and demonstrate that none of the bases are equivalent to each other under local unitaries. These bases are constructed from the continuous family of symmetric informationally complete sets of states in dimension three. By studying the local unitary bases that generate the family of two-qutrit maximally entangled measurement bases, we construct the first examples of wild error bases in the smallest dimension where these can exist. Finally, we discuss how distinct measurements in the family lead to differences in performance in several scenarios relevant in quantum information.Every two-qubit measurement basis composed of maximally entangled eigenstates can be transformed into the Bell basis via local unitary operations. For higher dimensions, in contrast, there exist inequivalent bases composed of maximally entangled eigenstates. Here, we provide a single-parameter family of two-qutrit maximally entangled measurement bases, and demonstrate that none of the bases are equivalent to each other under local unitaries. These bases are constructed from the continuous family of symmetric informationally complete sets of states in dimension three. By studying the local unitary bases that generate the family of two-qutrit maximally entangled measurement bases, we construct the first examples of wild error bases in the smallest dimension where these can exist. Finally, we discuss how distinct measurements in the family lead to differences in performance in several scenarios relevant in quantum information.

quant-pharXiv:2607.16396Jul 21, 20260 citations

Local unitary classification for sets of generalized Bell states

Bujiao Wu, Jiaqing Jiang, Jialin Zhang +2 more

In this paper, we study the local unitary (LU) classification for pairs (triples) of generalized Bell states, based on the local unitary equivalence of two sets. In detail, we first introduce some general unitary operators which give us more local unitary equivalent sets besides Clifford operators. And then we present two necessary conditions for local unitary equivalent sets which can be used to examine the local inequivalence. Following this approach, we completely classify all pairs in the $d\ensuremath{\bigotimes}d$ quantum system into ${\ensuremath{\prod}}_{j=1}^{n}({k}_{j}+1)\ensuremath{-}1$ LU-inequivalent pairs when the prime factorization of $d={\ensuremath{\prod}}_{j=1}^{n}{p}_{j}^{{k}_{j}}$. Moreover, all triples in the ${p}^{\ensuremath{\alpha}}\ensuremath{\bigotimes}{p}^{\ensuremath{\alpha}}$ quantum system for prime $p$ can be partitioned into $\frac{(\ensuremath{\alpha}+3)}{6}{p}^{\ensuremath{\alpha}}+O(\ensuremath{\alpha}{p}^{\ensuremath{\alpha}\ensuremath{-}1})$ LU-inequivalent triples; especially, when $\ensuremath{\alpha}=2$ and $p>2$ , there are exactly $\ensuremath{\lfloor}\frac{5}{6}{p}^{2}\ensuremath{\rfloor}+\ensuremath{\lfloor}\frac{p\ensuremath{-}2}{6}+{(\ensuremath{-}1)}^{\ensuremath{\lfloor}\frac{p}{3}\ensuremath{\rfloor}}\frac{p}{3}\ensuremath{\rfloor}+3$ LU-inequivalent triples.In this paper, we study the local unitary (LU) classification for pairs (triples) of generalized Bell states, based on the local unitary equivalence of two sets. In detail, we first introduce some general unitary operators which give us more local unitary equivalent sets besides Clifford operators. And then we present two necessary conditions for local unitary equivalent sets which can be used to examine the local inequivalence. Following this approach, we completely classify all pairs in the $d\ensuremath{\bigotimes}d$ quantum system into ${\ensuremath{\prod}}_{j=1}^{n}({k}_{j}+1)\ensuremath{-}1$ LU-inequivalent pairs when the prime factorization of $d={\ensuremath{\prod}}_{j=1}^{n}{p}_{j}^{{k}_{j}}$. Moreover, all triples in the ${p}^{\ensuremath{\alpha}}\ensuremath{\bigotimes}{p}^{\ensuremath{\alpha}}$ quantum system for prime $p$ can be partitioned into $\frac{(\ensuremath{\alpha}+3)}{6}{p}^{\ensuremath{\alpha}}+O(\ensuremath{\alpha}{p}^{\ensuremath{\alpha}\ensuremath{-}1})$ LU-inequivalent triples; especially, when $\ensuremath{\alpha}=2$ and $p>2$, there are exactly $\ensuremath{\lfloor}\frac{5}{6}{p}^{2}\ensuremath{\rfloor}+\ensuremath{\lfloor}\frac{p\ensuremath{-}2}{6}+{(\ensuremath{-}1)}^{\ensuremath{\lfloor}\frac{p}{3}\ensuremath{\rfloor}}\frac{p}{3}\ensuremath{\rfloor}+3$ LU-inequivalent triples.

arXiv:1711.06026Physical Review AAug 3, 201814 citations

p

can be partitioned into $\frac{(\ensuremath{\alpha}+3)}{6}{p}^{\ensuremath{\alpha}}+O(\ensuremath{\alpha}{p}^{\ensuremath{\alpha}\ensuremath{-}1})$ LU-inequivalent triples; especially, when $\ensuremath{\alpha}=2$ and

p>2

, there are exactly $\ensuremath{\lfloor}\frac{5}{6}{p}^{2}\ensuremath{\rfloor}+\ensuremath{\lfloor}\frac{p\ensuremath{-}2}{6}+{(\ensuremath{-}1)}^{\ensuremath{\lfloor}\frac{p}{3}\ensuremath{\rfloor}}\frac{p}{3}\ensuremath{\rfloor}+3$ LU-inequivalent triples.