Weak value

We will denote the initial state of a system as ${\displaystyle |\psi _{i}\rangle }$, while the final state of the system is denoted as ${\displaystyle |\psi _{f}\rangle }$. We will refer to the initial and final states of the system as the pre- and post-selected quantum mechanical states. With respect to these states, the weak value of the observable ${\displaystyle A}$ is defined as:

$${\displaystyle A_{w}={\frac {\langle \psi _{f}|A|\psi _{i}\rangle }{\langle \psi _{f}|\psi _{i}\rangle }}.}$$

Notice that if ${\displaystyle |\psi _{f}\rangle =|\psi _{i}\rangle }$ then the weak value is equal to the usual expected value in the initial state ${\displaystyle \langle \psi _{i}|A|\psi _{i}\rangle }$ or the final state ${\displaystyle \langle \psi _{f}|A|\psi _{f}\rangle }$. In general the weak value quantity is a complex number. The weak value of the observable becomes large when the post-selected state, ${\displaystyle |\psi _{f}\rangle }$, approaches being orthogonal to the pre-selected state, ${\displaystyle |\psi _{i}\rangle }$, i.e. ${\displaystyle |\langle \psi _{f}|\psi _{i}\rangle |\ll 1}$. If ${\displaystyle A_{w}}$ is larger than the largest eigenvalue of ${\displaystyle A}$ or smaller than the smallest eigenvalue of ${\displaystyle A}$ the weak value is said to be anomalous.

As an example consider a spin 1/2 particle.[8] Take ${\displaystyle A}$ to be the Pauli Z operator ${\displaystyle A=\sigma _{z}}$ with eigenvalues ${\displaystyle \pm 1}$. Using the initial state

$${\displaystyle |\psi _{i}\rangle ={\frac {1}{\sqrt {2}}}{\begin{pmatrix}\cos {\frac {\alpha }{2}}+\sin {\frac {\alpha }{2}}\\\cos {\frac {\alpha }{2}}-\sin {\frac {\alpha }{2}}\end{pmatrix}}}$$

and the final state

$${\displaystyle |\psi _{f}\rangle ={\frac {1}{\sqrt {2}}}{\begin{pmatrix}1\\1\end{pmatrix}}}$$

we can calculate the weak value to be

$${\displaystyle A_{w}=(\sigma _{z})_{w}=\tan {\frac {\alpha }{2}}.}$$

For ${\displaystyle |\alpha |>{\frac {\pi }{2}}}$ the weak value is anomalous.

Here we follow the presentation given by Duck, Stevenson, and Sudarshan,[8] (with some notational updates from Kofman et al.[4] )which makes explicit when the approximations used to derive the weak value are valid.

Consider a quantum system that you want to measure by coupling an ancillary (also quantum) measuring device. The observable to be measured on the system is ${\displaystyle A}$. The system and ancilla are coupled via the Hamiltonian

$${\displaystyle H=\gamma A\otimes p,}$$

where the coupling constant is integrated over an interaction time ${\textstyle \gamma =\int _{t_{i}}^{t_{f}}g(t)dt\ll 1}$ and ${\displaystyle [q,p]=i}$ is the canonical commutator. The Hamiltonian generates the unitary

$${\displaystyle U=\exp[-i\gamma A\otimes p].}$$

Take the initial state of the ancilla to have a Gaussian distribution

$${\displaystyle |\Phi \rangle ={\frac {1}{(2\pi \sigma ^{2})^{1/4}}}\int dq'\exp[-q'^{2}/4\sigma ^{2}]|q'\rangle ,}$$

the position wavefunction of this state is

$${\displaystyle \Phi (q)=\langle q|\Phi \rangle ={\frac {1}{(2\pi \sigma ^{2})^{1/4}}}\exp[-q^{2}/4\sigma ^{2}].}$$

The initial state of the system is given by ${\displaystyle |\psi _{i}\rangle }$ above; the state ${\displaystyle |\Psi \rangle }$, jointly describing the initial state of the system and ancilla, is given then by:

$${\displaystyle |\Psi \rangle =|\psi _{i}\rangle \otimes |\Phi \rangle .}$$

Next the system and ancilla interact via the unitary ${\displaystyle U|\Psi \rangle }$. After this one performs a projective measurement of the projectors ${\displaystyle \{|\psi _{f}\rangle \langle \psi _{f}|,I-|\psi _{f}\rangle \langle \psi _{f}|\}}$ on the system. If we postselect (or condition) on getting the outcome ${\displaystyle |\psi _{f}\rangle \langle \psi _{f}|}$, then the (unnormalized) final state of the meter is

$${\displaystyle {\begin{aligned}|\Phi _{f}\rangle &=\langle \psi _{f}|U|\psi _{i}\rangle \otimes |\Phi \rangle \\&\approx \langle \psi _{f}|(I\otimes I-i\gamma A\otimes p)|\psi _{i}\rangle \otimes |\Phi \rangle \quad {\text{(I)}}\\&=\langle \psi _{f}|\psi _{i}\rangle (1-i\gamma A_{w}p)|\Phi \rangle \\&\approx \langle \psi _{f}|\psi _{i}\rangle \exp(-i\gamma A_{w}p)|\Phi \rangle .\quad {\text{(II)}}\end{aligned}}}$$

To arrive at this conclusion, we use the first order series expansion of ${\displaystyle U}$ on line (I), and we require that[4][8]

$${\displaystyle {\begin{aligned}{\frac {|\gamma |}{\sigma }}\left|{\frac {\langle \psi _{f}|A^{n}|\psi _{i}\rangle }{\langle \psi _{f}|A|\psi _{i}\rangle }}\right|^{1/(n-1)}\ll 1,\quad (n=2,3,\dots )\end{aligned}}}$$

On line (II) we use the approximation that ${\displaystyle e^{-x}\approx 1-x}$ for small ${\displaystyle x}$. This final approximation is only valid when[4][8]

$${\displaystyle |\gamma A_{w}|/\sigma \ll 1.}$$

As ${\displaystyle p}$ is the generator of translations, the ancilla's wavefunction is now given by

$${\displaystyle \Phi _{f}(q)=\Phi (q-\gamma A_{w}).}$$

This is the original wavefunction, shifted by an amount ${\displaystyle \gamma A_{w}}$. By Busch's theorem[9] the system and meter wavefunctions are necessarily disturbed by the measurement. There is a certain sense in which the protocol that allows one to measure the weak value is minimally disturbing,[10] but there is still disturbance.[10]

At the end of the original weak value paper[1] the authors suggested weak values could be used in quantum metrology:

This suggestion was followed by Hosten and Kwiat[11] and later by Dixon et al.[12] It appears to be an interesting line of research that could result in improved quantum sensing technology.

Additionally in 2011, weak measurements of many photons prepared in the same pure state, followed by strong measurements of a complementary variable, were used to perform quantum tomography (i.e. reconstruct the state in which the photons were prepared).[13]

Weak values have been used to examine some of the paradoxes in the foundations of quantum theory. This relies to a large extent on whether weak values are deemed to be relevant to describe properties of quantum systems,[14] a point which is not obvious since weak values are generally different from eigenvalues. For example, the research group of Aephraim M. Steinberg at the University of Toronto confirmed Hardy's paradox experimentally using joint weak measurement of the locations of entangled pairs of photons.[15][16] (also see[17])

Building on weak measurements, Howard M. Wiseman proposed a weak value measurement of the velocity of a quantum particle at a precise position, which he termed its "naïvely observable velocity". In 2010, a first experimental observation of trajectories of a photon in a double-slit interferometer was reported, which displayed the qualitative features predicted in 2001 by Partha Ghose[18] for photons in the de Broglie-Bohm interpretation.[19][20] Following up on Wiseman's weak velocity measurement, Johannes Fankhauser and Patrick Dürr suggest in a paper that weak velocity measurements constitute no new arguments, let alone empirical evidence, in favor of or against standard de Broglie-Bohm theory. According to the authors such measurements could not provide direct experimental evidence displaying the shape of particle trajectories, even if it is assumed that some deterministic particle trajectories exist.[21]

Weak values have been implemented into quantum computing to get a giant speed up in time complexity. In a paper,[22] Arun Kumar Pati describes a new kind of quantum computer using weak value amplification and post-selection (WVAP), and implements search algorithm which (given a successful post selection) can find the target state in a single run with time complexity ${\displaystyle O(\log N)}$, beating out the well known Grover's algorithm.