- Source: Separable state
In quantum mechanics, separable states are multipartite quantum states that can be written as a convex combination of product states. Product states are multipartite quantum states that can be written as a tensor product of states in each space. The physical intuition behind these definitions is that product states have no correlation between the different degrees of freedom, while separable states might have correlations, but all such correlations can be explained as due to a classical random variable, as opposed as being due to entanglement.
In the special case of pure states the definition simplifies: a pure state is separable if and only if it is a product state.
A state is said to be entangled if it is not separable. In general, determining if a state is separable is not straightforward and the problem is classed as NP-hard.
Separability of bipartite systems
Consider first composite states with two degrees of freedom, referred to as bipartite states. By a postulate of quantum mechanics these can be described as vectors in the tensor product space
H
1
⊗
H
2
{\displaystyle H_{1}\otimes H_{2}}
. In this discussion we will focus on the case of the Hilbert spaces
H
1
{\displaystyle H_{1}}
and
H
2
{\displaystyle H_{2}}
being finite-dimensional.
= Pure states
=Let
{
|
a
i
⟩
}
i
=
1
n
⊂
H
1
{\displaystyle \{|{a_{i}}\rangle \}_{i=1}^{n}\subset H_{1}}
and
{
|
b
j
⟩
}
j
=
1
m
⊂
H
2
{\displaystyle \{|{b_{j}}\rangle \}_{j=1}^{m}\subset H_{2}}
be orthonormal bases for
H
1
{\displaystyle H_{1}}
and
H
2
{\displaystyle H_{2}}
, respectively. A basis for
H
1
⊗
H
2
{\displaystyle H_{1}\otimes H_{2}}
is then
{
|
a
i
⟩
⊗
|
b
j
⟩
}
{\displaystyle \{|{a_{i}}\rangle \otimes |{b_{j}}\rangle \}}
, or in more compact notation
{
|
a
i
b
j
⟩
}
{\displaystyle \{|a_{i}b_{j}\rangle \}}
. From the very definition of the tensor product, any vector of norm 1, i.e. a pure state of the composite system, can be written as
|
ψ
⟩
=
∑
i
,
j
c
i
,
j
(
|
a
i
⟩
⊗
|
b
j
⟩
)
=
∑
i
,
j
c
i
,
j
|
a
i
b
j
⟩
,
{\displaystyle |\psi \rangle =\sum _{i,j}c_{i,j}(|a_{i}\rangle \otimes |b_{j}\rangle )=\sum _{i,j}c_{i,j}|a_{i}b_{j}\rangle ,}
where
c
i
,
j
{\displaystyle c_{i,j}}
is a constant.
If
|
ψ
⟩
{\displaystyle |\psi \rangle }
can be written as a simple tensor, that is, in the form
|
ψ
⟩
=
|
ψ
1
⟩
⊗
|
ψ
2
⟩
{\displaystyle |\psi \rangle =|\psi _{1}\rangle \otimes |\psi _{2}\rangle }
with
|
ψ
i
⟩
{\displaystyle |\psi _{i}\rangle }
a pure state in the i-th space, it is said to be a product state, and, in particular, separable. Otherwise it is called entangled. Note that, even though the notions of product and separable states coincide for pure states, they do not in the more general case of mixed states.
Pure states are entangled if and only if their partial states are not pure. To see this, write the Schmidt decomposition of
|
ψ
⟩
{\displaystyle |\psi \rangle }
as
|
ψ
⟩
=
∑
k
=
1
r
ψ
p
k
(
|
u
k
⟩
⊗
|
v
k
⟩
)
,
{\displaystyle |\psi \rangle =\sum _{k=1}^{r_{\psi }}{\sqrt {p_{k}}}(|u_{k}\rangle \otimes |v_{k}\rangle ),}
where
p
k
>
0
{\displaystyle {\sqrt {p_{k}}}>0}
are positive real numbers,
r
ψ
{\displaystyle r_{\psi }}
is the Schmidt rank of
|
ψ
⟩
{\displaystyle |\psi \rangle }
, and
{
|
u
k
⟩
}
k
=
1
r
ψ
⊂
H
1
{\displaystyle \{|u_{k}\rangle \}_{k=1}^{r_{\psi }}\subset H_{1}}
and
{
|
v
k
⟩
}
k
=
1
r
ψ
⊂
H
2
{\displaystyle \{|v_{k}\rangle \}_{k=1}^{r_{\psi }}\subset H_{2}}
are sets of orthonormal states in
H
1
{\displaystyle H_{1}}
and
H
2
{\displaystyle H_{2}}
, respectively.
The state
|
ψ
⟩
{\displaystyle |\psi \rangle }
is entangled if and only if
r
ψ
>
1
{\displaystyle r_{\psi }>1}
. At the same time, the partial state has the form
ρ
A
≡
Tr
B
(
|
ψ
⟩
⟨
ψ
|
)
=
∑
k
=
1
r
ψ
p
k
|
u
k
⟩
⟨
u
k
|
.
{\displaystyle \rho _{A}\equiv \operatorname {Tr} _{B}(|\psi \rangle \!\langle \psi |)=\sum _{k=1}^{r_{\psi }}p_{k}\,|u_{k}\rangle \!\langle u_{k}|.}
It follows that
ρ
A
{\displaystyle \rho _{A}}
is pure --- that is, is projection with unit-rank --- if and only if
r
ψ
=
1
{\displaystyle r_{\psi }=1}
, which is equivalent to
|
ψ
⟩
{\displaystyle |\psi \rangle }
being separable.
Physically, this means that it is not possible to assign a definite (pure) state to the subsystems, which instead ought to be described as statistical ensembles of pure states, that is, as density matrices. A pure state
ρ
=
|
ψ
⟩
⟨
ψ
|
{\displaystyle \rho =|\psi \rangle \!\langle \psi |}
is thus entangled if and only if the von Neumann entropy of the partial state
ρ
A
≡
Tr
B
(
ρ
)
{\displaystyle \rho _{A}\equiv \operatorname {Tr} _{B}(\rho )}
is nonzero.
Formally, the embedding of a product of states into the product space is given by the Segre embedding. That is, a quantum-mechanical pure state is separable if and only if it is in the image of the Segre embedding.
For example, in a two-qubit space, where
H
1
=
H
2
=
C
2
{\displaystyle H_{1}=H_{2}=\mathbb {C} ^{2}}
, the states
|
0
⟩
⊗
|
0
⟩
{\displaystyle |0\rangle \otimes |0\rangle }
,
|
0
⟩
⊗
|
1
⟩
{\displaystyle |0\rangle \otimes |1\rangle }
,
|
1
⟩
⊗
|
1
⟩
{\displaystyle |1\rangle \otimes |1\rangle }
, are all product (and thus separable) pure states, as is
|
0
⟩
⊗
|
ψ
⟩
{\displaystyle |0\rangle \otimes |\psi \rangle }
with
|
ψ
⟩
≡
1
/
3
|
0
⟩
+
2
/
3
|
1
⟩
{\displaystyle |\psi \rangle \equiv {\sqrt {1/3}}|0\rangle +{\sqrt {2/3}}|1\rangle }
. On the other hand, states like
1
/
2
|
00
⟩
+
1
/
2
|
11
⟩
{\displaystyle {\sqrt {1/2}}|00\rangle +{\sqrt {1/2}}|11\rangle }
or
1
/
3
|
01
⟩
+
2
/
3
|
10
⟩
{\displaystyle {\sqrt {1/3}}|01\rangle +{\sqrt {2/3}}|10\rangle }
are not separable.
= Mixed states
=Consider the mixed state case. A mixed state of the composite system is described by a density matrix
ρ
{\displaystyle \rho }
acting on
H
1
⊗
H
2
{\displaystyle H_{1}\otimes H_{2}}
. Such a state
ρ
{\displaystyle \rho }
is separable if there exist
p
k
≥
0
{\displaystyle p_{k}\geq 0}
,
{
ρ
1
k
}
{\displaystyle \{\rho _{1}^{k}\}}
and
{
ρ
2
k
}
{\displaystyle \{\rho _{2}^{k}\}}
which are mixed states of the respective subsystems such that
ρ
=
∑
k
p
k
ρ
1
k
⊗
ρ
2
k
{\displaystyle \rho =\sum _{k}p_{k}\rho _{1}^{k}\otimes \rho _{2}^{k}}
where
∑
k
p
k
=
1.
{\displaystyle \;\sum _{k}p_{k}=1.}
Otherwise
ρ
{\displaystyle \rho }
is called an entangled state. We can assume without loss of generality in the above expression that
{
ρ
1
k
}
{\displaystyle \{\rho _{1}^{k}\}}
and
{
ρ
2
k
}
{\displaystyle \{\rho _{2}^{k}\}}
are all rank-1 projections, that is, they represent pure ensembles of the appropriate subsystems. It is clear from the definition that the family of separable states is a convex set.
Notice that, again from the definition of the tensor product, any density matrix, indeed any matrix acting on the composite state space, can be trivially written in the desired form, if we drop the requirement that
{
ρ
1
k
}
{\displaystyle \{\rho _{1}^{k}\}}
and
{
ρ
2
k
}
{\displaystyle \{\rho _{2}^{k}\}}
are themselves states and
∑
k
p
k
=
1.
{\displaystyle \;\sum _{k}p_{k}=1.}
If these requirements are satisfied, then we can interpret the total state as a probability distribution over uncorrelated product states.
In terms of quantum channels, a separable state can be created from any other state using local actions and classical communication while an entangled state cannot.
When the state spaces are infinite-dimensional, density matrices are replaced by positive trace class operators with trace 1, and a state is separable if it can be approximated, in trace norm, by states of the above form.
If there is only a single non-zero
p
k
{\displaystyle p_{k}}
, then the state can be expressed just as
ρ
=
ρ
1
⊗
ρ
2
,
{\textstyle \rho =\rho _{1}\otimes \rho _{2},}
and is called simply separable or product state. One property of the product state is that in terms of entropy,
S
(
ρ
)
=
S
(
ρ
1
)
+
S
(
ρ
2
)
.
{\displaystyle S(\rho )=S(\rho _{1})+S(\rho _{2}).}
Extending to the multipartite case
The above discussion generalizes easily to the case of a quantum system consisting of more than two subsystems. Let a system have n subsystems and have state space
H
=
H
1
⊗
⋯
⊗
H
n
{\displaystyle H=H_{1}\otimes \cdots \otimes H_{n}}
. A pure state
|
ψ
⟩
∈
H
{\displaystyle |\psi \rangle \in H}
is separable if it takes the form
|
ψ
⟩
=
|
ψ
1
⟩
⊗
⋯
⊗
|
ψ
n
⟩
.
{\displaystyle |\psi \rangle =|\psi _{1}\rangle \otimes \cdots \otimes |\psi _{n}\rangle .}
Similarly, a mixed state ρ acting on H is separable if it is a convex sum
ρ
=
∑
k
p
k
ρ
1
k
⊗
⋯
⊗
ρ
n
k
.
{\displaystyle \rho =\sum _{k}p_{k}\rho _{1}^{k}\otimes \cdots \otimes \rho _{n}^{k}.}
Or, in the infinite-dimensional case, ρ is separable if it can be approximated in the trace norm by states of the above form.
Separability criterion
The problem of deciding whether a state is separable in general is sometimes called the separability problem in quantum information theory. It is considered to be a difficult problem. It has been shown to be NP-hard in many cases and is believed to be so in general. Some appreciation for this difficulty can be obtained if one attempts to solve the problem by employing the direct brute force approach, for a fixed dimension. The problem quickly becomes intractable, even for low dimensions. Thus more sophisticated formulations are required. The separability problem is a subject of current research.
A separability criterion is a necessary condition a state must satisfy to be separable. In the low-dimensional (2 X 2 and 2 X 3) cases, the Peres-Horodecki criterion is actually a necessary and sufficient condition for separability. Other separability criteria include (but not limited to) the range criterion, reduction criterion, and those based on uncertainty relations. See Ref. for a review of separability criteria in discrete variable systems.
In continuous variable systems, the Peres-Horodecki criterion also applies. Specifically, Simon formulated a particular version of the Peres-Horodecki criterion in terms of the second-order moments of canonical operators and showed that it is necessary and sufficient for
1
⊕
1
{\displaystyle 1\oplus 1}
-mode Gaussian states (see Ref. for a seemingly different but essentially equivalent approach). It was later found that Simon's condition is also necessary and sufficient for
1
⊕
n
{\displaystyle 1\oplus n}
-mode Gaussian states, but no longer sufficient for
2
⊕
2
{\displaystyle 2\oplus 2}
-mode Gaussian states. Simon's condition can be generalized by taking into account the higher order moments of canonical operators or by using entropic measures.
Characterization via algebraic geometry
Quantum mechanics may be modelled on a projective Hilbert space, and the categorical product of two such spaces is the Segre embedding. In the bipartite case, a quantum state is separable if and only if it lies in the image of the Segre embedding.
Jon Magne Leinaas, Jan Myrheim and Eirik Ovrum in their paper "Geometrical aspects of entanglement" describe the problem and study the geometry of the separable states as a subset of the general state matrices. This subset have some intersection with the subset of states holding Peres-Horodecki criterion. In this paper, Leinaas et al. also give a numerical approach to test for separability in the general case.
Testing for separability
Testing for separability in the general case is an NP-hard problem. Leinaas et al. formulated an iterative, probabilistic algorithm for testing if a given state is separable. When the algorithm is successful, it gives an explicit, random, representation of the given state as a separable state. Otherwise it gives the distance of the given state from the nearest separable state it can find.
See also
Entanglement witness
References
External links
"StateSeparator" web-app
Kata Kunci Pencarian:
- BM-30 Smerch
- Karl-Anthony Towns
- Separable state
- Separable verb
- Entanglement witness
- Quantum entanglement
- Entropy of entanglement
- Multipartite entanglement
- No-cloning theorem
- Quantum metrological gain
- Mathematical formulation of quantum mechanics
- Modal verb
