Quantum state

Probability densities for the electron of a hydrogen atom in different quantum states.

In the mathematical formulation of quantum mechanics, pure quantum states correspond to vectors in a Hilbert space, while each observable quantity (such as the energy or momentum of a particle) is associated with a mathematical operator. The operator serves as a linear function which acts on the states of the system. The eigenvalues of the operator correspond to the possible values of the observable. For example, it is possible to observe a particle with a momentum of 1 kg⋅m/s if and only if one of the eigenvalues of the momentum operator is 1 kg⋅m/s. The corresponding eigenvector (which physicists call an eigenstate) with eigenvalue 1 kg⋅m/s would be a quantum state with a definite, well-defined value of momentum of 1 kg⋅m/s, with no quantum uncertainty. If its momentum were measured, the result is guaranteed to be 1 kg⋅m/s.

On the other hand, a system in a superposition of multiple different eigenstates does in general have quantum uncertainty for the given observable. We can represent this linear combination of eigenstates as:

${\displaystyle |\Psi (t)\rangle =\sum _{n}C_{n}(t)|\Phi _{n}\rangle .}$

The coefficient which corresponds to a particular state in the linear combination is a complex number, thus allowing interference effects between states. The coefficients are time dependent. How a quantum state changes in time is governed by the time evolution operator. The symbols ${\displaystyle |}$ and ${\displaystyle \rangle }$[lower-alpha 1] surrounding the ${\displaystyle \Psi }$ are part of bra–ket notation.

Statistical mixtures of states are a different type of linear combination. A statistical mixture of states is a statistical ensemble of independent systems. Statistical mixtures represent the degree of knowledge whilst the uncertainty within quantum mechanics is fundamental. Mathematically, a statistical mixture is not a combination using complex coefficients, but rather a combination using real-valued, positive probabilities of different states ${\displaystyle \Phi _{n}}$. A number ${\displaystyle P_{n}}$ represents the probability of a randomly selected system being in the state ${\displaystyle \Phi _{n}}$. Unlike the linear combination case each system is in a definite eigenstate.[7][8]

The expectation value ${\displaystyle \langle A\rangle _{\sigma }}$ of an observable A is a statistical mean of measured values of the observable. It is this mean, and the distribution of probabilities, that is predicted by physical theories.

There is no state which is simultaneously an eigenstate for all observables. For example, we cannot prepare a state such that both the position measurement Q(t) and the momentum measurement P(t) (at the same time t) are known exactly; at least one of them will have a range of possible values.[lower-alpha 2] This is the content of the Heisenberg uncertainty relation.

Moreover, in contrast to classical mechanics, it is unavoidable that performing a measurement on the system generally changes its state.[9][10][lower-alpha 3] More precisely: After measuring an observable A, the system will be in an eigenstate of A; thus the state has changed, unless the system was already in that eigenstate. This expresses a kind of logical consistency: If we measure A twice in the same run of the experiment, the measurements being directly consecutive in time,[lower-alpha 4] then they will produce the same results. This has some strange consequences, however, as follows.

Consider two incompatible observables, A and B, where A corresponds to a measurement earlier in time than B.[lower-alpha 5] Suppose that the system is in an eigenstate of B at the experiment's beginning. If we measure only B, all runs of the experiment will yield the same result. If we measure first A and then B in the same run of the experiment, the system will transfer to an eigenstate of A after the first measurement, and we will generally notice that the results of B are statistical. Thus: Quantum mechanical measurements influence one another, and the order in which they are performed is important.

Another feature of quantum states becomes relevant if we consider a physical system that consists of multiple subsystems; for example, an experiment with two particles rather than one. Quantum physics allows for certain states, called entangled states, that show certain statistical correlations between measurements on the two particles which cannot be explained by classical theory. For details, see entanglement. These entangled states lead to experimentally testable properties (Bell's theorem) that allow us to distinguish between quantum theory and alternative classical (non-quantum) models.

One can take the observables to be dependent on time, while the state σ was fixed once at the beginning of the experiment. This approach is called the Heisenberg picture. (This approach was taken in the later part of the discussion above, with time-varying observables P(t), Q(t).) One can, equivalently, treat the observables as fixed, while the state of the system depends on time; that is known as the Schrödinger picture. (This approach was taken in the earlier part of the discussion above, with a time-varying state ${\textstyle |\Psi (t)\rangle =\sum _{n}C_{n}(t)|\Phi _{n}\rangle }$.) Conceptually (and mathematically), the two approaches are equivalent; choosing one of them is a matter of convention.

Both viewpoints are used in quantum theory. While non-relativistic quantum mechanics is usually formulated in terms of the Schrödinger picture, the Heisenberg picture is often preferred in a relativistic context, that is, for quantum field theory. Compare with Dirac picture.[12]^:65

Quantum physics is most commonly formulated in terms of linear algebra, as follows. Any given system is identified with some finite- or infinite-dimensional Hilbert space. The pure states correspond to vectors of norm 1. Thus the set of all pure states corresponds to the unit sphere in the Hilbert space, because the unit sphere is defined as the set of all vectors with norm 1.

Multiplying a pure state by a scalar is physically inconsequential (as long as the state is considered by itself). If a vector in a complex Hilbert space ${\displaystyle H}$ can be obtained from another vector by multiplying by some non-zero complex number, the two vectors are said to correspond to the same "ray" in ${\displaystyle H}$[1]^:50 and also to the same point in the projective Hilbert space of ${\displaystyle H}$.

Calculations in quantum mechanics make frequent use of linear operators, scalar products, dual spaces and Hermitian conjugation. In order to make such calculations flow smoothly, and to make it unnecessary (in some contexts) to fully understand the underlying linear algebra, Paul Dirac invented a notation to describe quantum states, known as bra–ket notation. Although the details of this are beyond the scope of this article, some consequences of this are:

• The expression used to denote a state vector (which corresponds to a pure quantum state) takes the form ${\displaystyle |\psi \rangle }$ (where the "${\displaystyle \psi }$" can be replaced by any other symbols, letters, numbers, or even words). This can be contrasted with the usual mathematical notation, where vectors are usually lower-case latin letters, and it is clear from the context that they are indeed vectors.
• Dirac defined two kinds of vector, bra and ket, dual to each other.[lower-alpha 6]
• Each ket ${\displaystyle |\psi \rangle }$ is uniquely associated with a so-called bra, denoted ${\displaystyle \langle \psi |}$, which corresponds to the same physical quantum state. Technically, the bra is the adjoint of the ket. It is an element of the dual space, and related to the ket by the Riesz representation theorem. In a finite-dimensional space with a chosen basis, writing ${\displaystyle |\psi \rangle }$ as a column vector, ${\displaystyle \langle \psi |}$ is a row vector; to obtain it just take the transpose and entry-wise complex conjugate of ${\displaystyle |\psi \rangle }$.
• Scalar products[lower-alpha 7][lower-alpha 8] (also called brackets) are written so as to look like a bra and ket next to each other: ${\displaystyle \langle \psi _{1}|\psi _{2}\rangle }$. (The phrase "bra-ket" is supposed to resemble "bracket".)

The angular momentum has the same dimension (M·L²·T⁻¹) as the Planck constant and, at quantum scale, behaves as a discrete degree of freedom of a quantum system. Most particles possess a kind of intrinsic angular momentum that does not appear at all in classical mechanics and arises from Dirac's relativistic generalization of the theory. Mathematically it is described with spinors. In non-relativistic quantum mechanics the group representations of the Lie group SU(2) are used to describe this additional freedom. For a given particle, the choice of representation (and hence the range of possible values of the spin observable) is specified by a non-negative number S that, in units of Planck's reduced constant ħ, is either an integer (0, 1, 2 ...) or a half-integer (1/2, 3/2, 5/2 ...). For a massive particle with spin S, its spin quantum number m always assumes one of the 2S + 1 possible values in the set

${\displaystyle \{-S,-S+1,\ldots +S-1,+S\}}$

As a consequence, the quantum state of a particle with spin is described by a vector-valued wave function with values in C^2S+1. Equivalently, it is represented by a complex-valued function of four variables: one discrete quantum number variable (for the spin) is added to the usual three continuous variables (for the position in space).

The quantum state of a system of N particles, each potentially with spin, is described by a complex-valued function with four variables per particle, corresponding to 3 spatial coordinates and spin, e.g.

${\displaystyle |\psi (\mathbf {r} _{1},\,m_{1};\;\dots$ ;\;\mathbf {r} _{N},\,m_{N})\rangle .}

Here, the spin variables m_ν assume values from the set

${\displaystyle \{-S_{\nu },\,-S_{\nu }+1,\,\ldots ,\,+S_{\nu }-1,\,+S_{\nu }\}}$

where ${\displaystyle S_{\nu }}$ is the spin of νth particle. ${\displaystyle S_{\nu }=0}$ for a particle that does not exhibit spin.

The treatment of identical particles is very different for bosons (particles with integer spin) versus fermions (particles with half-integer spin). The above N-particle function must either be symmetrized (in the bosonic case) or anti-symmetrized (in the fermionic case) with respect to the particle numbers. If not all N particles are identical, but some of them are, then the function must be (anti)symmetrized separately over the variables corresponding to each group of identical variables, according to its statistics (bosonic or fermionic).

Electrons are fermions with S = 1/2, photons (quanta of light) are bosons with S = 1 (although in the vacuum they are massless and can't be described with Schrödinger mechanics).

When symmetrization or anti-symmetrization is unnecessary, N-particle spaces of states can be obtained simply by tensor products of one-particle spaces, to which we will return later.

As with any Hilbert space, if a basis is chosen for the Hilbert space of a system, then any ket can be expanded as a linear combination of those basis elements. Symbolically, given basis kets ${\displaystyle |{k_{i}}\rangle }$, any ket ${\displaystyle |\psi \rangle }$ can be written

${\displaystyle |\psi \rangle =\sum _{i}c_{i}|{k_{i}}\rangle }$

where c_i are complex numbers. In physical terms, this is described by saying that ${\displaystyle |\psi \rangle }$ has been expressed as a quantum superposition of the states ${\displaystyle |{k_{i}}\rangle }$. If the basis kets are chosen to be orthonormal (as is often the case), then ${\displaystyle c_{i}=\langle {k_{i}}|\psi \rangle }$.

One property worth noting is that the normalized states ${\displaystyle |\psi \rangle }$ are characterized by

${\displaystyle \langle \psi |\psi \rangle =1,}$

and for orthonormal basis this translates to

${\displaystyle \sum _{i}\left|c_{i}\right|^{2}=1.}$

Expansions of this sort play an important role in measurement in quantum mechanics. In particular, if the ${\displaystyle |{k_{i}}\rangle }$ are eigenstates (with eigenvalues k_i) of an observable, and that observable is measured on the normalized state ${\displaystyle |\psi \rangle }$, then the probability that the result of the measurement is k_i is |c_i|². (The normalization condition above mandates that the total sum of probabilities is equal to one.)

A particularly important example is the position basis, which is the basis consisting of eigenstates ${\displaystyle |\mathbf {r} \rangle }$ with eigenvalues ${\displaystyle \mathbf {r} }$ of the observable which corresponds to measuring position.[lower-alpha 9] If these eigenstates are nondegenerate (for example, if the system is a single, spinless particle), then any ket ${\displaystyle |\psi \rangle }$ is associated with a complex-valued function of three-dimensional space

${\displaystyle \psi (\mathbf {r} )\equiv \langle \mathbf {r} |\psi \rangle .}$[lower-alpha 11] i.e. ${\displaystyle \langle \mathbf {r} |\mathbf {r} '\rangle =\delta (\mathbf {r} '-\mathbf {r} )}$ (a Dirac delta function), which means that ${\displaystyle \langle \mathbf {r} |\mathbf {r} \rangle =\infty .}$</ref>

This function is called the wave function corresponding to ${\displaystyle |\psi \rangle }$. Similarly to the discrete case above, the probability density of the particle being found at position ${\displaystyle \mathbf {r} }$ is ${\displaystyle |\psi (\mathbf {r} )|^{2}}$ and the normalized states have

${\displaystyle \int \mathrm {d} ^{3}\mathbf {r} \,|\psi (\mathbf {r} )|^{2}=1}$.

In terms of the continuous set of position basis ${\displaystyle |\mathbf {r} \rangle }$, the state ${\displaystyle |\psi \rangle }$ is:

${\displaystyle |\psi \rangle =\int \mathrm {d} ^{3}\mathbf {r} \,\psi (\mathbf {r} )|\mathbf {r} \rangle }$.

As mentioned above, quantum states may be superposed. If ${\displaystyle |\alpha \rangle }$ and ${\displaystyle |\beta \rangle }$ are two kets corresponding to quantum states, the ket

${\displaystyle c_{\alpha }|\alpha \rangle +c_{\beta }|\beta \rangle }$

is a different quantum state (possibly not normalized). Note that both the amplitudes and phases (arguments) of ${\displaystyle c_{\alpha }}$ and ${\displaystyle c_{\beta }}$ will influence the resulting quantum state. In other words, for example, even though ${\displaystyle |\psi \rangle }$ and ${\displaystyle e^{i\theta }|\psi \rangle }$ (for real θ) correspond to the same physical quantum state, they are not interchangeable, since ${\displaystyle |\phi \rangle +|\psi \rangle }$ and ${\displaystyle |\phi \rangle +e^{i\theta }|\psi \rangle }$ will not correspond to the same physical state for all choices of ${\displaystyle |\phi \rangle }$. However, ${\displaystyle |\phi \rangle +|\psi \rangle }$ and ${\displaystyle e^{i\theta }(|\phi \rangle +|\psi \rangle )}$ will correspond to the same physical state. This is sometimes described by saying that "global" phase factors are unphysical, but "relative" phase factors are physical and important.

One practical example of superposition is the double-slit experiment, in which superposition leads to quantum interference. The photon state is a superposition of two different states, one corresponding to the photon travel through the left slit, and the other corresponding to travel through the right slit. The relative phase of those two states depends on the difference of the distances from the two slits. Depending on that phase, the interference is constructive at some locations and destructive in others, creating the interference pattern. We may say that superposed states are in coherent superposition, by analogy with coherence in other wave phenomena.

Another example of the importance of relative phase in quantum superposition is Rabi oscillations, where the relative phase of two states varies in time due to the Schrödinger equation. The resulting superposition ends up oscillating back and forth between two different states.

A pure quantum state is a state which can be described by a single ket vector, as described above. A mixed quantum state is a statistical ensemble of pure states (see quantum statistical mechanics). Mixed states inevitably arise from pure states when, for a composite quantum system ${\displaystyle H_{1}\otimes H_{2}}$ with an entangled state on it, the part ${\displaystyle H_{2}}$ is inaccessible to the observer. The state of the part ${\displaystyle H_{1}}$ is expressed then as the partial trace over ${\displaystyle H_{2}}$.

A mixed state cannot be described with a single ket vector. Instead, it is described by its associated density matrix (or density operator), usually denoted ρ. Note that density matrices can describe both mixed and pure states, treating them on the same footing. Moreover, a mixed quantum state on a given quantum system described by a Hilbert space ${\displaystyle H}$ can be always represented as the partial trace of a pure quantum state (called a purification) on a larger bipartite system ${\displaystyle H\otimes K}$ for a sufficiently large Hilbert space ${\displaystyle K}$.

The density matrix describing a mixed state is defined to be an operator of the form

${\displaystyle \rho =\sum _{s}p_{s}|\psi _{s}\rangle \langle \psi _{s}|}$

where ${\displaystyle p_{s}}$ is the fraction of the ensemble in each pure state ${\displaystyle |\psi _{s}\rangle .}$ The density matrix can be thought of as a way of using the one-particle formalism to describe the behavior of many similar particles by giving a probability distribution (or ensemble) of states that these particles can be found in.

A simple criterion for checking whether a density matrix is describing a pure or mixed state is that the trace of ρ² is equal to 1 if the state is pure, and less than 1 if the state is mixed.[lower-alpha 12][13] Another, equivalent, criterion is that the von Neumann entropy is 0 for a pure state, and strictly positive for a mixed state.

The rules for measurement in quantum mechanics are particularly simple to state in terms of density matrices. For example, the ensemble average (expectation value) of a measurement corresponding to an observable A is given by

${\displaystyle \langle A\rangle =\sum _{s}p_{s}\langle \psi _{s}|A|\psi _{s}\rangle =\sum _{s}\sum _{i}p_{s}a_{i}|\langle \alpha _{i}|\psi _{s}\rangle |^{2}=\operatorname {tr} (\rho A)}$

where ${\displaystyle |\alpha _{i}\rangle ,\;a_{i}}$ are eigenkets and eigenvalues, respectively, for the operator A, and "tr" denotes trace. It is important to note that two types of averaging are occurring, one being a weighted quantum superposition over the basis kets ${\displaystyle |\psi _{s}\rangle }$ of the pure states, and the other being a statistical (said incoherent) average with the probabilities p_s of those states.

According to Eugene Wigner,[14] the concept of mixture was put forward by Lev Landau.[15][16]^:38–41