Macroscopic quantum phenomena

Macroscopic quantum phenomena

Quantum mechanics is most often used to describe matter on the scale of molecules, atoms, or elementary particles. However, some phenomena, particularly at low temperatures, show quantum behavior on a macroscopic scale. The best-known examples of macroscopic quantum phenomena are superfluidity and superconductivity; another example is the quantum Hall effect. Since 2000 there has been extensive experimental work on quantum gases, particularly Bose–Einstein Condensates.

Between 1996 to 2003 four Nobel prizes were given for work related to macroscopic quantum phenomena.[1] Macroscopic quantum phenomena can be observed in superfluid helium and in superconductors,[2] but also in dilute quantum gases and in laser light. Although these media are very different, their behavior is very similar as they all show macroscopic quantum behavior.

Quantum phenomena are generally classified as macroscopic when the quantum states are occupied by a large number of particles (typically Avogadro's number) or the quantum states involved are macroscopic in size (up to km size in superconducting wires).

Consequences of the macroscopic occupation

Fig.1 Left: only one particle; usually the small box is empty. However, there is a certain chance of that the particle is in the box. This chance is given by Eq.(15). Middle: a few particles. There are usually some particles in the box. We can define an average, but the actual number of particles in the box has large fluctuations around this average. Right: large number of particles. The fluctuations around the average are small.

The concept of macroscopically-occupied quantum states is introduced by Fritz London.[3][4] In this section it will be explained what it means if the ground state is occupied by a very large number of particles. We start with the wave function of the ground state written as

\Psi = \Psi _0 \exp(i\varphi) (13)

with Ψ₀ the amplitude and \varphi the phase. The wave function is normalized so that

\int \Psi \Psi ^* \mathrm{d}V = N_s. (14)

The physical interpretation of the quantity

\Psi \Psi ^* \Delta V (15)

depends on the number of particles. Fig.1 represents a container with a certain number of particles with a small control volume ΔV inside. We check from time to time how many particles are in the control box. We distinguish three cases:

1. There is only one particle. In this case the control volume is empty most of the time. However, there is a certain chance to find the particle in it given by Eq.(15). The chance is proportional to ΔV. The factor ΨΨ is called the chance density.

2. If the number of particles is a bit larger there are usually some particles inside the box. We can define an average, but the actual number of particles in the box has relatively large fluctuations around this average.

3. In the case of a very large number of particles there will always be a lot of particles in the small box. The number will fluctuate but the fluctuations around the average are relatively small. The average number is proportional to ΔV and ΨΨ is now interpreted as the particle density.

In quantum mechanics the particle probability flow density Jp (unit: particles per second per m²) can be derived from the Schrödinger equation to be

\vec{J}_p = \frac{1}{2m}\left(\Psi (i \frac{h}{2\pi}\vec{\nabla} -q \vec{A})\Psi^* +cc \right) (16)

with q the charge of the particle and \vec{A} the vector potential. With Eq.(13)

\vec{J}_p = \frac {\Psi_0^2}{m}\left(\frac{h}{2 \pi} \vec{\nabla} \varphi - q \vec{A}\right). (17)

If the wave function is macroscopically occupied the particle probability flow density becomes a particle flow density. We introduce the fluid velocity vs via the mass flow density

m\vec{J}_p=\rho _s \vec{v}_s. (18)

The density (mass per m³) is

m \Psi_0^2 = \rho_s (19)

so Eq.(17) results in

\vec{v}_s=\frac{1}{m}\left(\frac{h}{2\pi}\vec{\nabla}\varphi-q\vec{A}\right). (20)

This important relation connects the velocity, a classical concept, of the condensate with the phase of the wave function, a quantum-mechanical concept.


Fig.2 Lower part: vertical cross section of a column of superfluid helium rotating around a vertical axis. Upper part: Top view of the surface showing the pattern of vortex cores. From left to right the rotation speed is increased resulting in an increasing vortex-line density.

Below the lambda-temperature helium shows the unique property of superfluidity. The fraction of the liquid that forms the superfluid component is a macroscopic quantum fluid. The helium atom is a neutral particle so q=0. Furthermore the particle mass m=m₄ so Eq.(20) reduces to

\vec{v}_s=\frac{1}{m_4}\frac{h}{2\pi}\vec{\nabla}\varphi. (21)

For an arbitrary loop in the liquid this gives

\oint \vec{v}_s\cdot\vec{\mathrm{d}s}=\frac{h}{2\pi m_4} \oint \vec{\nabla}\varphi \cdot \vec{\mathrm{d}s}. (22)

Due to the single-valued nature of the wave function

\oint \vec{\nabla}\varphi \cdot \vec{\mathrm{d}s} = 2\pi n (23a)

with n integer, we have

\oint \vec{v}_s\cdot\vec{\mathrm{d}s} =\frac{h}{m_4}n. (23b)
The quantity
\kappa =\frac{h}{m_4}=1.0 \times 10^{-7} m^2/s (24)
is the quantum of circulation. For a circular motion with radius r
\oint \vec{v}_s\cdot\vec{\mathrm{d}s} =2\pi v_sr. (25)
In case of a single quantum (n=1)
v_s=\frac{1}{2\pi r}\kappa. (26)

When superfluid helium is put in rotation Eq.(25) will not be satisfied for all loops inside the liquid unless the rotation is organized around vortex lines as depicted in Fig.2. These lines have a vacuum core with a diameter of about 1 Å (which is smaller than the average particle distance). The superfluid helium rotates around the core with very high speeds. Just outside the core (r = 1 Å) the velocity is as large as 160 m/s. The cores of the vortex lines and the container rotate as a solid body around the rotation axes with the same angular velocity. The number of vortex lines increases with the angular velocity as shown in the upper half of the figure. Note that the two right figures both contain six vortex lines, but the lines are organized in different stable patterns.[5]


Fluxoid quantization

For superconductors the bosons involved are the so-called Cooper pairs which are quasiparticles formed by two electrons.[6] Hence m = 2me and q = -2e where me and e are the mass of an electron and the elementary charge. It follows from Eq.(20) that

2m_e \vec{v}_s=\frac{h}{2\pi}\vec{\nabla}\varphi+2e\vec{A}. (27)

Integrating Eq.(27) over a closed loop gives

2m_e\oint \vec{v}_s\cdot\vec{\mathrm{d}s} = \oint(\frac{h}{2\pi}\vec{\nabla}\varphi+2e\vec{A})\cdot\vec{\mathrm{d}s} (28)

As in the case of helium we define the vortex strength

\oint \vec{v}_s\cdot\vec{\mathrm{d}s} =\kappa (29)

and use the general relation

\oint \vec{A}\cdot\vec{\mathrm{d}s} = \Phi (30)

where Φ is the magnetic flux enclosed by the loop. The so-called fluxoid is defined by

\Phi_v=\Phi-\frac{2m_e}{2e}\kappa. (31)

In general the values of κ and Φ depend on the choice of the loop. Due to the single-valued nature of the wave function and Eq.(28) the fluxoid is quantized

\Phi_v = n\frac{h}{2e}. (32)

The unit of quantization is called the flux quantum

\Phi_0=\frac{h}{2e} = 2.067833758(46)\times 10^{-15} Wb. (33)

The flux quantum plays a very important role in superconductivity. The earth magnetic field is very small (about 50 μT), but it generates one flux quantum in an area of 6 by 6 μm. So, the flux quantum is very small. Yet it was measured to an accuracy of 9 digits as shown in Eq.(33). Nowadays the value given by Eq.(33) is exact by definition.

Fig. 3. Two superconducting rings in an applied magnetic field
a: thick superconducting ring. The integration loop is completely in the region with vs=0;
b: thick superconducting ring with a weak link. The integration loop is completely in the region with vs=0 except for a small region near the weak link.

In Fig. 3 two situations are depicted of superconducting rings in an external magnetic field. One case is a thick-walled ring and in the other case the ring is also thick-walled, but is interrupted by a weak link. In the latter case we will meet the famous Josephson relations. In both cases we consider a loop inside the material. In general a superconducting circulation current will flow in the material. The total magnetic flux in the loop is the sum of the applied flux Φa and the self-induced flux Φs induced by the circulation current

\Phi = \Phi_a + \Phi_s. (34)

Thick ring

The first case is a thick ring in an external magnetic field (Fig. 3a). The currents in a superconductor only flow in a thin layer at the surface. The thickness of this layer is determined by the so-called London penetration depth. It is of μm size or less. We consider a loop far away from the surface so that vs=0 everywhere so κ=0. In that case the fluxoid is equal to the magnetic flux (Φv=Φ). If vs=0 Eq.(27) reduces to

0=\frac{h}{2\pi}\vec{\nabla}{\varphi}+2e\vec{A}. (35)

Taking the rotation gives

0=\frac{h}{2\pi}\vec{\nabla} \times \vec{\nabla}\varphi + 2e \vec{\nabla}\times\vec{A}. (36)

Using the well-known relations \vec{\nabla} \times \vec{\nabla}\varphi =0 and \vec{\nabla}\times\vec{A}=\vec{B} shows that the magnetic field in the bulk of the superconductor is zero as well. So, for thick rings, the total magnetic flux in the loop is quantized according to

\Phi=n\Phi_0. (37)

Interrupted ring, weak links

Fig. 4. Schematic of a weak link carrying a superconducting current is. The voltage difference over the link is V. The phases of the superconducting wave functions at the left and right side are assumed to be constant (in space, not in time) with values of φ1 and φ2 respectively.

Weak links play a very important role in modern superconductivity. In most cases weak links are oxide barriers between two superconducting thin films, but it can also be a crystal boundary (in the case of high-Tc superconductors). A schematic representation is given in Fig. 4. Now consider the ring which is thick everywhere except for a small section where the ring is closed via a weak link (Fig. 3b). The velocity is zero except near the weak link. In these regions the velocity contribution to the total phase change in the loop is given by (with Eq.(27))

\Delta\varphi^*=-\frac{2\pi}{h}2m_e\int_\delta \vec{v}_s\cdot\vec{\mathrm{d}s}. (38)

The line integral is over the contact from one side to the other in such a way that the end points of the line are well inside the bulk of the superconductor where vs=0. So the value of the line integral is well-defined (e.g. independent of the choice of the end points). With Eqs.(31), (34), and (38)

\Phi_a+\Phi_s+\Phi_0\frac{\Delta\varphi^*}{2\pi}=n\Phi_0. (39)

Without proof we state that the supercurrent through the weak link is given by the so-called DC Josephson relation[7]

i_s = i_1\sin(\Delta\varphi^*). (40)

The voltage over the contact is given by the AC Josephson relation

V=\frac{1}{2\pi}\frac{h}{2e}\frac{\mathrm{d}\Delta\varphi^*}{\mathrm{d}t}. (41)

The names of these relations (DC and AC relations) are misleading since they both hold in DC and AC situations. In the steady state (constant \Delta\varphi^*) Eq.(41) shows that V=0 while a nonzero current flows through the junction. In the case of a constant applied voltage (voltage bias) Eq.(41) can be integrated easily and gives

\Delta\varphi^*=2\pi\frac{2eV}{h}t. (42)

Substitution in Eq.(40) gives

i_s=i_1\sin(2\pi\frac{2eV}{h}t). (43)

This is an AC current. The frequency

\nu=\frac{2eV}{h}=\frac{V}{\Phi_0} (44)

is called the Josephson frequency. One μV gives a frequency of about 500 MHz. By using Eq.(44) the flux quantum is determined with the high precision as given in Eq.(33).

The energy difference of a Cooper pair, moving from one side of the contact to the other, is ΔE = 2eV. With this expression Eq.(44) can be written as ΔE = which is the relation for the energy of a photon with frequency ν.

The AC Josephson relation (Eq.(41)) can be easily understood in terms of Newton's law, (or from one of the London equation's[8]). We start with Newton's law
\vec F = m \mathrm{d}\vec v_s/\mathrm{d}t.
Substituting the expression for the Lorentz force
\vec F = q(\vec E+\vec v_s\times \vec B)
and using the general expression for the co-moving time derivative
\mathrm{d}\vec v_s/\mathrm{d}t=\part \vec v_s/\part t + (1/2)\vec \nabla v_s^2-\vec v_s\times(\vec \nabla\times \vec v_s)
(q/m)(\vec E+\vec v_s\times \vec B)=\part \vec v_s/\part t + (1/2)\vec \nabla v_s^2-\vec v_s\times(\vec \nabla\times \vec v_s).
Eq.(20) gives
0=\vec\nabla\times\vec v_s + (q/m)\vec\nabla\times\vec A = \vec\nabla\times\vec v_s + (q/m)\vec B
(q/m)\vec E=\part \vec v_s/\part t+(1/2) \vec \nabla v_s^2.
Take the line integral of this expression. In the end points the velocities are zero so the ∇v2 term gives no contribution. Using
\int \vec E\cdot\mathrm{d}\vec l = -V
and Eq.(38), with q = -2e and m =2me, gives Eq.(41).


Fig. 5. Two superconductors connected by two weak links. A current and a magnetic field are applied.
Fig. 6. Dependence of the critical current of a DC-SQUID on the applied magnetic field
Figure 5 shows a so-called DC SQUID. It consists of two superconductors connected by two weak links. The fluxoid quantization of a loop through the two bulk superconductors and the two weak links demands
\Delta\varphi_a^*=\Delta\varphi^*_b+2\pi\frac{\Phi}{\Phi_0}+2\pi n. (45)
If the self-inductance of the loop can be neglected the magnetic flux in the loop Φ is equal to the applied flux
\Phi=\Phi_a=BA (46)
with B the magnetic field, applied perpendicular to the surface, and A the surface area of the loop. The total supercurrent is given by
i_s=i_1\sin(\Delta\varphi_a^*)+i_1\sin(\Delta\varphi_b^*). (47)
Substitution of Eq(45) in (47) gives
i_s=i_1\sin(\Delta\varphi_b^*+2\pi\frac{\Phi}{\Phi_0})+i_1\sin(\Delta\varphi_b^*). (48)
Using a well known geometrical formula we get
i_s=2i_1\sin(\Delta\varphi_b^*+\pi\frac{\Phi}{\Phi_0})\cos(\pi\frac{\Phi_a}{\Phi_0}). (49)
Since the sin-function can vary only between −1 and +1 a steady solution is only possible if the applied current is below a critical current given by
i_c=2i_1|\cos(\pi\frac{\Phi_a}{\Phi_0})|. (50)

Note that the critical current is periodic in the applied flux with period Φ₀. The dependence of the critical current on the applied flux is depicted in Fig. 6. It has a strong resemblance with the interference pattern generated by a laser beam behind a double slit. In practice the critical current is not zero at half integer values of the flux quantum of the applied flux. This is due to the fact that the self-inductance of the loop cannot be neglected.[9]

Type II superconductivity

Fig. 7. Magnetic flux lines penetrating a type-II superconductor. The currents in the superconducting material generate a magnetic field which, together with the applied field, result in bundles of quantized flux.

Abrikosov vortex lattice similar to the pattern shown in Fig. 2.[10] A cross section of the superconducting plate is given in Fig. 7. Far away from the plate the field is homogeneous, but in the material superconducting currents flow which squeeze the field in bundles of exactly one flux quantum. The typical field in the core is as big as 1 tesla. The currents around the vortex core flow in a layer of about 50 nm with current densities on the order of 15×1012 A/m². That corresponds with 15 million ampère in a wire of one mm².

Dilute quantum gases

The classical types of quantum systems, superconductors and superfluid helium, were discovered in the beginning of the 20th century. Near the end of the 20th century, scientists discovered how to create very dilute atomic or molecular gases, cooled first by laser cooling and then by evaporative cooling.[11] They are trapped using magnetic fields or optical dipole potentials in ultrahigh vacuum chambers. Isotopes which have been used include rubidium (Rb-87 and Rb-85), strontium (Sr-87, Sr-86, and Sr-84) potassium (K-39 and K-40), sodium (Na-23), lithium (Li-7 and Li-6), and hydrogen (H-1). The temperatures to which they can be cooled are as low as a few nanokelvin. The developments have been very fast in the past few years. A team of NIST and the University of Colorado has succeeded in creating and observing vortex quantization in these systems.[12] The concentration of vortices increases with the angular velocity of the rotation, similar to the case of superfluid helium and superconductivity.

See also

References and footnotes

  1. ^ These Nobel prizes were for the discovery of super-fluidity in helium-3 (1996), for the discovery of the fractional quantum Hall effect (1998), for the demonstration of Bose–Einstein condensation (2001), and for contributions to the theory of superconductivity and superfluidity (2003).
  2. ^ D.R. Tilley and J. Tilley, Superfluidity and Superconductivity, Adam Hilger, Bristol and New York, 1990
  3. ^ Fritz London Superfluids (London, Wiley, 1954-1964)
  4. ^ Gavroglu, K.; Goudaroulis, Y. (1988). "Understanding macroscopic quantum phenomena: The history of superfluidity 1941–1955". Annals of Science 45 (4): 367.  
  5. ^ E.J. Yarmchuk and R.E. Packard (1982). "Photographic studies of quantized vortex lines". J. Low Temp. Phys. 46 (5–6): 479.  
  6. ^ M. Tinkham (1975). Introduction to Superconductivity. McGraw-Hill. 
  7. ^ B.D. Josephson (1962). "Possible new effects in superconductive tunneling". Phys. Lett. 1 (7): 251–253.  
  8. ^  
  9. ^ A.TH.A.M. de Waele and R. de Bruyn Ouboter (1969). "Quantum-interference phenomena in point contacts between two superconductors". Physica 41 (2): 225–254.  
  10. ^ Essmann, U.; Träuble, H. (1967). "The direct observation of individual flux lines in type II superconductors". Physics Letters A 24 (10): 526.  
  11. ^ Anderson, M.H., Ensher, J.R., Matthews, M.R., Wieman, C.E., and Cornell, E.A. (1995). "Observation of Bose-Einstein Condensation in a Dilute Atomic Vapor". Science 269 (5221): 198–201.  
  12. ^ Schweikhard, V., Coddington, I., Engels, P., Tung, S., and Cornell, E.A. (2004). "Vortex-Lattice Dynamics in Rotating Spinor Bose-Einstein Condensates". Phys. Rev. Lett. 93 (3): 210403.