# 4.5: Force

- Page ID
- 3442

Skills to Develop

- Explain force and relativity

Force is a concept that is seldom needed in relativity, and that’s why this section is optional.

### Four-force

By analogy with Newtonian mechanics, we deﬁne a relativistic force vector

\[F = m\cdot a\]

where \(a\) is the acceleration four-vector (section 3.5) and \(m\) is the mass of a particle that has that acceleration as a result of the force \(F\). This is equivalent to

\[F = \frac{\mathrm{d} p}{\mathrm{d} \tau }\]

where \(p\) is the mass of the particle and \(τ\) its proper time. Since the timelike part of \(p\) is the particle’s mass-energy, the timelike component of the force is related to the power expended by the force. These deﬁnitions only work for massive particles, since for a massless particle we can’t deﬁne \(a\) or \(τ\). \(F\) has been deﬁned in terms of Lorentz invariants and four-vectors, and therefore it transforms as a god-fearing four-vector itself.

### The force measured by an observer

The trouble with all this is that \(F\) isn’t what we actually measure when we measure a force, except if we happen to be in a frame of reference that momentarily coincides with the rest frame of the particle. As with velocity and acceleration (section 3.7), we have a four-vector that has simple, standard transformation properties, but a diﬀerent \(F_o\), which is what is actually measured by the observer \(o\). It’s deﬁned as

\[F_o = \frac{\mathrm{d} p}{\mathrm{d} t }\]

with a \(dt\) in the denominator rather than a \(dτ\). In other words, it measures the rate of transfer of momentum according to the observer, whose time coordinate is \(t\), not \(τ\) — unless the observer happens to be moving along with the particle. Unlike the three-vectors \(v_o\) and \(a_o\), whose timelike components are zero by deﬁnition according to observer \(o\), \(F_o\) usually has a nonvanishing timelike component, which is the rate of change of the particle’s mass-energy, i.e., the power. We can refer to the spacelike part of \(F_o\) as the three-force.

The following two examples show that an object moving at relativistic speeds has less inertia in the transverse direction than in the longitudinal one. A corollary is that the three-acceleration need not be parallel to the three-force.

Example \(\PageIndex{1}\): Circular motion

For a particle in uniform circular motion, \(γ\) is constant, and we have

\[F_o = \frac{\mathrm{d} }{\mathrm{d} t }(m\gamma v) = m\gamma \frac{\mathrm{d} v}{\mathrm{d} t}\]

The particle’s mass-energy is constant, so the timelike component of \(F_o\) does happen to be zero in this example. In terms of the three-vectors \(v_o\) and \(a_o\) deﬁned in section 3.7, we have

\[F_o = m\gamma \frac{\mathrm{d} v_o}{\mathrm{d} t} = m\gamma a_o\]

which is greater than the Newtonian value by the factor \(γ\). As a practical example, in a cathode ray tube(CRT) such as the tube in an old-fashioned oscilloscope or television, a beam of electrons is accelerated upto relativistic speed. To paint a picture on the screen, the beam has to be steered by transverse forces, and since the deﬂection angles are small, the world-line of the beam is approximately that of uniform circular motion. The force required to deﬂect the beam is greater by a factor of \(γ\) than would have been expected according to Newton’s laws.

Example \(\PageIndex{2}\): Linear motion

For accelerated linear motion in the x direction, ignoring \(y\) and \(z\), we have a velocity vector

\[v = \frac{\mathrm{d} r}{\mathrm{d} \tau }\]

whose \(x\) component is \(γv\). Then

\[\begin{align*} F_{o,x} &= m\frac{\mathrm{d} (\gamma v)}{\mathrm{d} t}\\ &= m\frac{\mathrm{d} (\gamma )}{\mathrm{d} t}v + m\gamma \frac{\mathrm{d} v}{\mathrm{d} t}\\ &= m\frac{\mathrm{d} \gamma }{\mathrm{d} v}\frac{\mathrm{d} v}{\mathrm{d} t} + m\gamma a\\ &= m\left ( v^2 \gamma ^3 a + \gamma a \right )\\ &= ma\gamma ^3 \end{align*}\]

The particle’s apparent inertia is increased by a factor of \(γ^3\) due to relativity.

The results of above two examples can be combined as follows:

\[F_o = m\gamma a_{o,\perp } + m\gamma ^3 a_{o,\parallel }\]

where the subscripts \(\perp\) and \(\parallel\) refer to the parts of \(a_o\) perpendicular and parallel to \(v_o\).

### Transformation of the force measured by an observer

Deﬁne a frame of reference \(o\) for the inertial frame of reference of an observer who does happen to be moving along with the particle at a particular instant in time. Then \(t\) is the same as \(τ\), and \(F_o\) the same as \(F\). In this frame, the particle is momentarily at rest, so the work being done on it vanishes, and the timelike components of \(F_o\) and \(F\) are both zero.

Suppose we do a Lorentz transformation from o to a new frame \(o'\), and suppose the boost is parallel to \(F_o\) and \(F\) (which are both purely spatial in frame \(o\)). Call this direction \(x\). Then \(dp = (dp_t,dp_x) = (0,dp_x)\) transforms to \(dp' = (-γv dp_x,γ dp_x)\), so that \(F_{o',x} = dp'_x/dt' = (γ dp_x)/(γ dt) = F_{o,x}\). The two factors of \(γ\) cancel, and we ﬁnd that \(F_{o',x} = F_{o,x}\).

Now let’s do the case where the boost is in the \(y\) direction, perpendicular to the force. The Lorentz transformation doesn’t change \(dp_y\), so

\[\begin{align*} F_{o',y} &= \frac{\mathrm{d} p'_y}{\mathrm{d} t'}\\ &= \frac{\mathrm{d} p_y}{(\gamma \mathrm{d} t)}\\ &= \frac{F_{o',y}}{\gamma } \end{align*}\]

The summary of our results is as follows. Let \(F_o\) be the force acting on a particle, as measured in a frame instantaneously comoving with the particle. Then in a frame of reference moving relative to this one, we have

\[F_{o',\parallel } = F_{o,\parallel }\]

and

\[F_{o',\perp } = \frac{F_{o,\perp }}{\gamma }\]

where \(\parallel\) indicates the direction parallel to the relative velocity of the two frames, and \(\perp\) a direction perpendicular to it.

### Work

Consider the one-dimensional version of the three-force, \(F = dp/dt\). An advantantage of this quantity is that it allows us to use the Newtonian form of the (one-dimensional) work-kinetic energy relation \(dE/dx = F\) without correction. Proof:

\[\frac{\mathrm{d} E}{\mathrm{d} x} = \frac{\mathrm{d} E}{\mathrm{d} p} \frac{\mathrm{d} p}{\mathrm{d} t} \frac{\mathrm{d} t}{\mathrm{d} x} = \frac{\mathrm{d} E}{\mathrm{d} p} \frac{F}{v}\]

By implicit diﬀerentiation of the deﬁnition of mass, we ﬁnd that \(dE/dp = p/E\), and this in turn equals \(v\) by the identity proved in Example 4.3.2. This leads to the claimed result, which is valid for both massless and material particles.

### Contributors

- Benjamin Crowell (Fullerton College). Special Relativity is copyrighted with a CC-BY-SA license.