Symmetry-protected topological order

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Symmetry-protected topological (SPT) order^[1][2] is a kind of order in zero-temperature quantum-mechanical states of matter that have a symmetry and a finite energy gap.

To derive the results in a most-invariant way, renormalization group methods are used (leading to equivalence classes corresponding to certain fixed points).^[1] The SPT order has the following defining properties:

(a) distinct SPT states with a given symmetry cannot be smoothly deformed into each other without a phase transition, if the deformation preserves the symmetry.
(b) however, they all can be smoothly deformed into the same trivial product state without a phase transition, if the symmetry is broken during the deformation.

The above definition works for both bosonic systems and fermionic systems, which leads to the notions of bosonic SPT order and fermionic SPT order.

Using the notion of quantum entanglement, we can say that SPT states are states with a symmetry (by contrast: for long-range entanglement see topological order, which is not related to the famous EPR paradox). Since short-range entangled states have only trivial topological orders we may also refer the SPT order as Symmetry Protected "Trivial" order.

Characteristic properties[]

1. The boundary effective theory of a non-trivial SPT state always has pure gauge anomaly or mixed gauge-gravity anomaly for the symmetry group.^[3] As a result, the boundary of a SPT state is either gapless or degenerate, regardless how we cut the sample to form the boundary. A gapped non-degenerate boundary is impossible for a non-trivial SPT state. If the boundary is a gapped degenerate state, the degeneracy may be caused by spontaneous symmetry breaking and/or (intrinsic) topological order.
2. in non-trivial 2+1D SPT states carry non-trival statistics^[4] and fractional quantum numbers^[5] of the symmetry group. Monodromy defects are created by twisting the boundary condition along a cut by a symmetry transformation. The ends of such cut are the monodromy defects. For example, 2+1D bosonic Z_n SPT states are classified by a Z_n integer m. One can show that n identical elementary monodromy defects in a Z_n SPT state labeled by m will carry a total Z_n quantum number 2m which is not a multiple of n.
3. 2+1D bosonic U(1) SPT states have a Hall conductance that is quantized as an even integer.^[6][7] 2+1D bosonic SO(3) SPT states have a quantized spin Hall conductance.^[8]

Relation between SPT order and (intrinsic) topological order[]

SPT states are short-range entangled while topologically ordered states are long-range entangled. Both intrinsic topological order, and also SPT order, can sometimes have protected . The difference is subtle: the gapless boundary excitations in intrinsic topological order can be robust against any local perturbations, while the gapless boundary excitations in SPT order are robust only against local perturbations that do not break the symmetry. So the gapless boundary excitations in intrinsic topological order are topologically protected, while the gapless boundary excitations in SPT order are symmetry protected.^[9]

We also know that an intrinsic topological order has emergent fractional charge, emergent fractional statistics, and emergent gauge theory. In contrast, a SPT order has no emergent fractional charge/fractional statistics for finite-energy excitations, nor emergent gauge theory (due to its short-range entanglement). Note that the monodromy defects discussed above are not finite-energy excitations in the spectrum of the Hamiltonian, but defects created by modifying the Hamiltonian.

Examples[]

The first example of SPT order is the Haldane phase of odd-integer-spin chain.^{[10][11][12][13]} It is a SPT phase protected by SO(3) spin rotation symmetry.^[1] (Note that Haldane phases of even-integer-spin chain do not have SPT order.) A more well known example of SPT order is the topological insulator of non-interacting fermions, a SPT phase protected by U(1) and time reversal symmetry.

On the other hand, fractional quantum Hall states are not SPT states. They are states with (intrinsic) topological order and long-range entanglements.

Group cohomology theory for SPT phases[]

Using the notion of quantum entanglement, one obtains the following general picture of gapped phases at zero temperature. All gapped zero-temperature phases can be divided into two classes: phases (ie phases with intrinsic topological order) and phases (ie phases with no intrinsic topological order). All short-range entangled phases can be further divided into three classes: symmetry-breaking phases, SPT phases, and their mix (symmetry breaking order and SPT order can appear together).

It is well known that symmetry-breaking orders are described by group theory. For bosonic SPT phases with pure gauge anomalous boundary, it was shown that they are classified by group cohomology theory:^[14][15] those (d+1)D SPT states with symmetry G are labeled by the elements in group cohomology class ${\displaystyle H^{d+1}[G,U(1)]}$. For other (d+1)D SPT states^{[16] [17] [18] [19]} with mixed gauge-gravity anomalous boundary, they can be described by ${\displaystyle \oplus _{k=1}^{d}H^{k}[G,iTO^{d+1-k}]}$,^[20] where ${\displaystyle iTO^{d+1}}$ is the Abelian group formed by (d+1)D topologically ordered phases that have no non-trivial topological excitations (referred as iTO phases).

From the above results, many new quantum states of matter are predicted, including bosonic topological insulators (the SPT states protected by U(1) and time-reversal symmetry) and bosonic topological superconductors (the SPT states protected by time-reversal symmetry), as well as many other new SPT states protected by other symmetries.

A list of bosonic SPT states from group cohomology ${\displaystyle H^{d+1}[G,U(1)]\oplus _{k=1}^{d}H^{k}[G,iTO^{d+1-k}]}$ (${\displaystyle Z_{2}^{T}}$ = time-reversal-symmetry group)

symmetry group	1+1D	2+1D	3+1D	4+1D	comment
${\displaystyle 0}$	${\displaystyle 0}$	${\displaystyle Z}$	${\displaystyle 0}$	${\displaystyle Z_{2}}$	iTO phases with no symmetry: ${\displaystyle iTO^{d+1}}$
${\displaystyle U(1)\rtimes Z_{2}^{T}}$	${\displaystyle Z_{2}}$	${\displaystyle Z_{2}}$	${\displaystyle 2Z_{2}+Z_{2}}$	${\displaystyle Z\oplus Z_{2}+Z}$	bosonic topological insulator
${\displaystyle Z_{2}^{T}}$	${\displaystyle Z_{2}}$	${\displaystyle 0}$	${\displaystyle Z_{2}+Z_{2}}$	${\displaystyle 0}$	bosonic topological superconductor
${\displaystyle Z_{n}}$	${\displaystyle 0}$	${\displaystyle Z_{n}}$	${\displaystyle 0}$	${\displaystyle Z_{n}+Z_{n}}$
${\displaystyle U(1)}$	${\displaystyle 0}$	${\displaystyle Z}$	${\displaystyle 0}$	${\displaystyle Z+Z}$	2+1D: quantum Hall effect
${\displaystyle SO(3)}$	${\displaystyle Z_{2}}$	${\displaystyle Z}$	${\displaystyle 0}$	${\displaystyle Z_{2}}$	1+1D: odd-integer-spin chain; 2+1D: spin Hall effect
${\displaystyle SO(3)\times Z_{2}^{T}}$	${\displaystyle 2Z_{2}}$	${\displaystyle Z_{2}}$	${\displaystyle 3Z_{2}+Z_{2}}$	${\displaystyle 2Z_{2}}$
${\displaystyle Z_{2}\times Z_{2}\times Z_{2}^{T}}$	${\displaystyle 4Z_{2}}$	${\displaystyle 6Z_{2}}$	${\displaystyle 9Z_{2}+Z_{2}}$	${\displaystyle 12Z_{2}+2Z_{2}}$

The phases before "+" come from ${\displaystyle H^{d+1}[G,U(1)]}$. The phases after "+" come from ${\displaystyle \oplus _{k=1}^{d}H^{k}[G,iTO^{d+1-k}]}$. Just like group theory can give us 230 crystal structures in 3+1D, group cohomology theory can give us various SPT phases in any dimensions with any on-site symmetry groups.

On the other hand, the fermionic SPT orders are described by theory.^[21] So the group (super-)cohomology theory allows us to construct many SPT orders even for interacting systems, which include interacting topological insulator/superconductor.

A complete classification of 1D gapped quantum phases (with interactions)[]

Using the notions of quantum entanglement and SPT order, one can obtain a complete classification of all 1D gapped quantum phases.

First, it is shown that there is no (intrinsic) topological order in 1D (ie all 1D gapped states are short-range entangled).^[22] Thus, if the Hamiltonians have no symmetry, all their 1D gapped quantum states belong to one phase—the phase of trivial product states. On the other hand, if the Hamiltonians do have a symmetry, their 1D gapped quantum states are either symmetry-breaking phases, SPT phases, and their mix.

Such an understanding allows one to classify all 1D gapped quantum phases:^{[14][23][24][25][26]} All 1D gapped phases are classified by the following three mathematical objects: ${\displaystyle (G_{H},G_{\Psi },H^{2}[G_{\Psi },U(1)])}$ , where ${\displaystyle G_{H}}$ is the symmetry group of the Hamiltonian, ${\displaystyle G_{\Psi }}$ the symmetry group of the ground states, and ${\displaystyle H^{2}[G_{\Psi },U(1)]}$ the second group cohomology class of ${\displaystyle G_{\Psi }}$. (Note that ${\displaystyle H^{2}[G,U(1)]}$ classifies the projective representations of ${\displaystyle G}$.) If there is no symmetry breaking (ie ${\displaystyle G_{\Psi }=G_{H}}$), the 1D gapped phases are classified by the projective representations of symmetry group ${\displaystyle G_{H}}$.

See also[]

• AKLT Model
• Topological insulator
• Quantum spin Hall effect
• Topological order

References[]